Released this past November, the list is based on data collected from the Web of Science and highlights some of the world’s most influential scientific minds by naming the researchers whose publications over the previous decade have included a high number of Highly Cited Papers placing them among the top 1% most-cited.
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We wish to congratulate all of the researchers named and especially our authors on this amazing accomplishment! We are happy and proud to share in their success!
IntechOpen is proud to announce that 179 of our authors have made the Clarivate™ Highly Cited Researchers List for 2020, ranking them among the top 1% most-cited.
\n\n
Throughout the years, the list has named a total of 252 IntechOpen authors as Highly Cited. Of those researchers, 69 have been featured on the list multiple times.
\n\n\n\n
Released this past November, the list is based on data collected from the Web of Science and highlights some of the world’s most influential scientific minds by naming the researchers whose publications over the previous decade have included a high number of Highly Cited Papers placing them among the top 1% most-cited.
\n\n
We wish to congratulate all of the researchers named and especially our authors on this amazing accomplishment! We are happy and proud to share in their success!
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\r\n\tWeather warnings released all over the world as well as the regional level even on the country level, which is important forecasts. They use it to protect life and property. The weather forecasting is playing an important role in planning and management to save the infrastructure and people's lives from disasters. Weather forecasting determines the atmosphere process in the future. It is related to understanding the atmospheric process through observed and remote sensing meteorology data. We can say the collecting as much as data as possible about the current state of the atmosphere particularly the temperature, humidity, and wind. There is a vast variety of end uses to weather forecasts. There is a number of methods i.e. statistically, numerical, artificial neural network, and different weather forecasting models. Climate change increases the demand for weather forecasting. Due to weather forecasts, decision-makers can take different protective measures in every field of life especially agriculture regarding food hunger. The extreme event of weather impact on agriculture as well as infrastructure.
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1. Introduction
The topology of electronic band structures in crystals can have profound consequences at their interfaces with materials having a trivial topology, resulting in novel electronic states in reduced dimension [1, 2]. A striking example is the realization of gapless metallic states with a Dirac band structure at the interface between two insulators, if one is a topological insulator (TI). For a 2D crystal, these are dissipationless 1D spin-helical edge states, an electronic phase known as the quantum spin Hall state [3, 4, 5]. For a 3D crystal, the metallic phase develops as 2D surface/interface states [6, 7] with a spin-helical band structure that limits their scattering by non-magnetic disorder [8]. This novel type of insulators was discovered in materials having a strong spin-orbit coupling (broken rotational symmetry) and a Hamiltonian invariant by time-reversal symmetry (TRS), belonging to the so-called ℤ2 topological class [7, 9]. The spin-orbit interaction can lead to a band inversion that gives rise to novel quasi-particles having a Dirac-like band structure with spin-momentum locking, at the interface with a trivial insulator (i.e., with non-inverted bands) where the energy gap must close (see Figure 1a). A remarkable property is that such metallic states always exist (no gap), even in the presence of perturbations, as long as the main symmetries are preserved. Thus, regardless the strength of a non-magnetic disorder, the condition for strong (Anderson) localization is never fulfilled. Still, an electronic gap (an important property for the operation of classical electronic devices) can be created, for instance by using a perturbation breaking TRS or by coupling topological states at opposite interfaces. The non-trivial nature of such gapped topological states further gives rise to novel exotic phases with a lower dimension (Majorana bound states [10] and quantum anomalous Hall state [11]) of particular interest for the quantum manipulation of coherent states weakly coupled to their environment.
Figure 1.
(a) Evolution of the band gap between a trivial insulator and a 3D topological insulator (with an inverted bulk band structure). At the interface, the gap closes and metallic states with a linear dispersion form. (b) These interface/surface states are 2D spin-helical Dirac fermions, with opposite spin helicity for opposite surfaces (the simplest case of a single Dirac cone in the center of the Brillouin zone is sketched).
The importance of topological insulators also comes from that they represent a promising alternative to conventional semi-conducting hetero-structures with, in principle, a reduced complexity on the materials’ side and an increased stability of their electronic phases (over a large range of physical parameters: temperature, magnetic field, chemical potential, and disorder/inhomogeneities). The most striking example came with the discovery of the quantum spin Hall edge states in a 2D topological insulator, first evidenced with HgCdTe quantum wells [12]. This novel electronic phase shares some similarities with the magnetic-field induced integer quantum Hall state in high-mobility low-density 2D electron gases (2DEGs) of massive quasi-particles but was predicted in zero field [3, 4, 13] (no magnetic-field induced orbital effect). Another important discovery was that of 3D topological insulators [14, 15, 16], which realize a 2D electron gas of massless Dirac fermions (different from those in graphene due to their helical spin texture) at the surfaces/interfaces of a single crystalline film (Figure 1b), whereas the creation of a charge-accumulation 2D gas of massive quasi-particles in conventional semiconductors often requires a more complex stacking of epitaxial layers of materials with different energy gaps and electronic-band offsets. In practice, the control of surface electronic states in a 3D topological insulator also requires that of band bending at interfaces (due to charge transfer from the environment) and a significant limitation to investigate topological surface-state transport came from that most materials are not true bulk insulators. Still, an important difference with massive quasi-particles in semiconductors, or Dirac fermions in graphene, is the reduced scattering rate by disorder due to the spin-helical texture of surface Dirac fermions [8, 17]. This favors the quasi-ballistic transport of such quasi-particles, even if they directly coexist with a large density of scattering centers, and it gives a new possibility to study such a transport regime [18] that is otherwise only accessible for massive quasi-particles in rather high-mobility AlGaAs 2DEGs (for which the 2DEG is spatially separated from Coulomb scatterers). Besides, the spin-momentum locking property of the Dirac cone favors the efficient spin-charge conversion in spintronic devices [19, 20, 21, 22, 23, 24, 25], still with some potential for improvement due to the enhanced transport length [17], if interface scattering could be further reduced.
Contrary to the case of 2D TIs, with only rare examples found to date, a number of 3D TI materials were discovered, both by theory and experiments, often using ab initio calculations or electron spectroscopy techniques to directly unveil the Dirac band structure of topological surface states (TSS). This offered an important playground to investigate [26, 27], but it is also a source of confusion due to the diversity of these materials and the complexity of some of them. In particular, their study by charge transport measurements proved to be difficult because many materials identified as topological insulators are also semiconductors with a rather small gap, often with a large finite bulk conductivity due to disorder (electrical doping) and a strong electronic polarizability [28]. The search for large-gap 3D topological insulators remains challenging. Indeed, beyond the need for specific symmetries of the crystal structure, it is fundamental to search for materials with a band inversion. With conventional semiconductors, this inversion is usually induced by a strong intrinsic spin-orbit coupling. This is typical for materials with large-Z elements, which also have a rather small bulk energy gap induced by Coulomb interactions. This combination is therefore favorable to realize a band inversion, and since it results from opposite contributions, most Z2 topological insulators tend to have a rather small gap that barely exceeds 300 meV in most cases. Natural point defects, such as vacancies (which are thermodynamically stable and therefore always exist in crystals), can be massively present (small activation energy) and they often act as donors or acceptors, thus easily leading to metallic-like bulk properties typical of degenerate semiconductors (sometimes approaching the dirty-metal limit). Among these semiconductors, Bi-based chalcogenides play an important role for that the continuous tuning of their chemical composition, between different stoichiometric compounds, can change a trivial insulator (no band inversion) into a topological insulator (band inversion), with a varying bulk gap and a relative change of the topological Dirac degeneracy point with respect to the bulk band structure [29]. Binary 3D topological insulators, such as Bi2Se3 and Bi2Te3, usually have a large residual bulk conductivity (despite a very small bulk-carrier mobility), so that the total conductance of wide and/or thick nanostructures is dominated by bulk transport. This contribution is slightly reduced in Bi2Te3, but only high-energy surface quasi-particles can be studied because the Dirac point lies deep into the valence band, whereas the Fermi level is pinned near or above the top of the valence band. In Bi2Se3, the Dirac point lies within the bulk band gap, but the Fermi level is high above the bottom of the conduction band (due to too many Se vacancies), so that it can only be modified over a small energy range by an electrical gate (efficient electrostatic screening), unless the nanostructure is ultra thin. Ternary compounds gave the most advanced results to optimize the surface-to-bulk ratio to the conductance and this approach was successfully used to investigate surface-state transport in the quantum Hall regime at low magnetic fields (close to the Dirac point) [30]. It remains, however, difficult to prepare nanostructures (thin films, nanoribbons, and nanowires) of ternary or even quaternary materials with optimized compositions [31]. Novel heterostructures, such as core-shell nanowires, could thus be important to develop functional devices based on 3D topological insulators, not only to achieve dominant surface transport and use the spin-momentum locking property of 2D topological surface states, but also to realize novel low-dimensional quantum devices at the sub-micron scale despite disorder, due to anisotropic scattering, which are different from “conventional” mesoscopic conductors with either massive quasi-particles in semiconductors or Dirac fermions in graphene (both with quantum transport properties controlled by large-angle scattering).
Unique properties of spin-helical Dirac fermions in disordered 3D topological insulators also arise from their strong quantum confinement in narrow nanowires (quantum wires). The Dirac nature results in a large energy quantization, as compared to the confinement energy of massive quasi-particles, which further reduces their scattering by disorder and favors the quasi-ballistic transport of quasi-1D surface modes [18]. Thus, their quantized band structure gives some specific signatures of topological surface-state transport, unveiled by quantum corrections to the conductance [18, 32, 33], which can be easily distinguished from bulk transport (even for highly-degenerate semiconductors, such as Bi2Se3 and Bi2Te3). Their spin texture also contribute to reduce their coupling to the environment, so that decoherence due to electronic interactions is also further reduced. All in all, 3D topological insulator quantum wires offer new possibilities to investigate mesoscopic transport in the quasi-ballistic regime over a large range of parameters (dimensionality, aspect ratio, and disorder strength), whereas it can hardly be investigated otherwise. Rare studies based on high-mobility AlGaAs 2DEGs were limited to the near-clean limit [34, 35], with little possibilities to modify some important physical parameters, such as disorder or the kinetic energy, over a broad range. Disordered semiconducting or metallic nanowires are always diffusive conductors. Disordered semiconducting or metallic nanowires are always diffusive conductors. Most similar systems are actually carbon nanotubes, which are clean systems with ballistic-transport properties and very large confinement energies. Disordered 3D TI quantum wires represent an intermediate situation that corresponds to quasi-ballistic transport (due to anisotropic scattering rather than to a weak disorder) and their quantized surface states can be manipulated with rather small magnetic fields, due to larger diameters than for carbon nanotubes. As a consequence, the specific properties of quantized surface Dirac modes can be revealed by the study of different quantum corrections to the conductance (Aharonov-Bohm oscillations and non-universal conductance fluctuations), with good statistical information obtained from magneto-transport measurements below 15 T [18].
2. Transport properties of 2D topological surface states
To understand the physics of 3DTI quantum wires, it is first necessary to take a closer look at the scattering of 2D spin-helical Dirac fermions by a non-magnetic disorder. In this case, backscattering is not suppressed since it remains possible by successive small-angle scattering events, over a scale given by the transport length, ltr. However, the spin texture favors forward scattering, so that the transport length of topological surface state is largely enhanced with respect to the disorder correlation length. As a consequence, the condition for ballistic transport can already be realized in nanostructures with dimensions smaller than a micron, and quantum devices with a simple geometry can be built from individual nanowires.
2.1. Nanostructures of 3D topological insulators for surface-transport studies
Due to their residual bulk doping, the study of surface-state transport in disordered 3D topological insulators is not straightforward. Considering the case of a highly-degenerate semiconductor, such as Bi2Se3, with a bulk carrier density as high as 5·1019 cm−3 (which roughly corresponds to about 1% of Se vacancies, acting as double donors), the cross over thickness tc for which the surface conductance becomes comparable to the bulk conductance is roughly given by tc = 2(nsμs)/(nbμb). For a strong disorder typical for Bi2Se3, common to both surface and bulk states, the mobility of topological surface states is about one order of magnitude larger than that of bulk states (enhancement due to the anisotropic scattering of spin-helical Dirac fermions) [17]. Taking band bending into account [36], typical values for the surface and bulk carrier densities are ns = 5·1012 cm−2 and nb = 5·1019 cm−3. This gives a value tc = 20 nm. Based on a realistic approximation (ignoring details of band bending due to a very short Thomas-Fermi screening length λTF ≲ 3 nm), this lower bound for tc (which is likely be larger for smaller bulk carrier densities) clearly shows that the control of topological surface-state transport in disordered 3D TIs requires the use of thin nanostructures. These were successfully grown by different bottom-up methods, each technique having both advantages and disadvantages. Ultra-thin layers of high quality can be prepared by molecular beam epitaxy and are well adapted to tune the interface band structure by electrical fields, but films thicker than 20 nm tend to grow 3D and have more defects. High-quality single-crystalline nanostructures with large aspect ratios can be grown by catalyst-assisted molecular-beam epitaxy or chemical vapor deposition, as well as by catalyst-free vapor transport, but ultra-thin structures are seldom. Very narrow quantum wires can also be prepared by electrodeposition in nanomembranes, presently with some intrinsic limitations related to small diameter fluctuations in ultimate nanomembranes that give quantum confinement inhomogeneities. In all cases, individual nanostructures stable in air can be randomly grown on or transferred onto SiOx/Si substrates, appropriate to create an electric field at the interface by applying a backgate voltage.
In our work, we mostly investigated the charge transport properties of single-crystalline atomic-flat Bi2Se3 and Bi2Te3 nanostructures grown by catalyst-free vapor transport (Figure 2a), with faceted shapes of different aspect ratios (nanoplatelets, nanoribbons, nanowires; Figure 2b) [37]. As explained below, this allowed us to study the physics of spin-helical Dirac fermions in 2D or in 1D, that is, without or with quantum confinement, respectively. Despite strong disorder, it was shown that momentum scattering is reduced in all cases, due to the spin texture (2D surface states) and quantum confinement (1D surface modes). This has important consequences for both spin transport and quantum coherent transport, as discussed in detail below.
Figure 2.
(a) Growth of Bi2Se3 nanostructures on p++-Si/SiO2 substrates by vapor transport in a closed quartz ampoule. The sublimation of Bi2Se3 crystals generates a flow of molecular species (BiSe and Se2) toward the lower temperature area, where the recombine to form single crystalline nanostructures in the plane of the substrate. (b) Nanostructures with different aspect ratios (thin platelets, wide nanoribbons, and narrow nanowires) are distributed randomly onto amorphous SiO2. After [37].
2.2. Band bending and interface charge transfers
The electrical properties of 2D topological surface states can be investigated by quantum magneto-transport G(B) studies and transconductance G(Vg) measurements at low temperatures, which give access to all microscopic parameters (carrier density, mobility, and effective mass) for all carriers (topological interface states, topological surface states, and bulk states). A careful analysis of Shubnikov-de Haas oscillations due to the energy quantization of Landau levels in high magnetic fields gave detailed insights into the electronic band profiles in the thickness of wide Bi2Se3 nanostructures (nanoplatelets and nanoribbons) [36]. Important results are summarized as follows:
Due to the large residual bulk density and the pinning of the Fermi energy in the conduction or valence band of materials with a large dielectric constant, the bulk contribution to the conductance is never negligible.
Besides, it usually controls the upward band bending at interfaces of the topological insulator (charge transfer of bulk carriers to empty gapless topological surface states).
Downward band bending can, however, exist if a massive charge transfer from another origin is also present (surface/interface disorder, surface adsorbents, and electrostatic gate). Such a situation is more likely to happen for materials with a small bulk carrier density.
If the surface/interface density is very large (typically for ns > 1013 cm−2), a Rashba charge-accumulation 2DEG of massive quasi-particles coexist with Dirac topological states.
For usual as-grown Bi2Se3 nanostructures exposed to air, a typical band profile is defined from the contribution of three electronic populations (bulk carriers and two topological states with different Fermi energies), and the bulk carrier density is large enough to control charge transfer at interfaces and to induce upward band bending. Due to efficient Coulomb screening, an electrostatic gate is solely influencing the population of a single topological interface nearby, so that an independent tuning of both topological states is only achieved in dual-gate devices [38]. In a backgate geometry, the applied voltage is modifying the band bending at the bottom interface only, which results in the tuning of the electro-chemical potential of the interface topological states but not of the surface topological states since, in most cases, the electrical field is totally screened by bulk carriers nearby the bottom interface [17]. In all cases, the backgate-voltage dependence of the conductance nevertheless remains an efficient way to probe the interface topological states and study their properties by transport measurements. A striking example is shown in Figure 3, for a rather thick Bi2Se3 nanoribbon patterned in a Hall-bar geometry, with a low-enough bulk-carrier density to favor downward band bending at interfaces [36]. For a large interface carrier density, massless Dirac fermions coexist with a Rashba-type massive 2D electron gas. In this case, the back-gate voltage is changing the carrier concentration of different electronic states located at the bottom interface (shift of some peaks in the Fourier transform of Shubnikov de Haas oscillations, Figure 3b). The related band profile shown in Figure 3c is in very good quantitative agreement with a triangular potential at this interface.
Figure 3.
(a) Scanning-electron microscope image of a Hall-bar patterned Bi2Se3 thick nanoribbons, (b) fast-Fourier transform of the longitudinal magneto-resistance for two different back-gate voltages, and (c) evolution of the electronic band profile from the top surface to the bottom interface, typical for a low bulk-carrier density (downward band bending) and a large interface carrier density (coexistence of topological states with a Rashba 2DEG). After [36].
2.3. Anisotropic scattering and charge transport length (=spin diffusion length)
Further important information on the scattering of spin-helical Dirac fermions by a non-magnetic disorder can be obtained from transconductance G(V_G) measurements [17]. It is indeed important to distinguish between two different scattering times and, accordingly, between two different length scales (Figure 4a):
The quantum lifetime of quasi-particles can be inferred from Shubnikov-de Hass measurements. It is associated with the mean-free path le between two successive scattering centers (thus to the microscopic disorder correlation length) and this momentum scattering time relates to the quantum mobility.
The transport time of carriers corresponds to the timescale for momentum backscattering, over a length called the transport length Ltr, related to the transport mobility, which determines the classical conductance. Whereas direct backscattering is forbidden by spin-momentum locking (giving dissipationless states in a 2D TI), it is allowed by multiple scattering processes in a disordered 3D TI, resulting in a finite transport length.
Figure 4.
(a) Anisotropic scattering by disorder. The backscattering transport length Ltr can be much longer than the mean-free path le; (b) scanning electron microscope image of a thin Bi2Se3 nanoribbon with traversing ohmic contacts; (c) longitudinal magneto-conductance for two different backgate voltages. Inset: Shubnikov-de Haas quantum oscillations; (d) backgate voltage dependence of the conductance and linear fit from which the transport length of the lower surface states (bottom interface) is inferred. After [17].
Using a thin Bi2Se3 nanoribbon (Figure 4b), the backgate voltage allowed us to modify the upward band bending, induced by a rather large bulk carrier density, at the bottom interface (“lower surface state”, LSS). All microscopic transport parameters could be inferred from quantum magneto-transport (Figure 4c) and trans-conductance (Figure 4d) measurements [17]. Contrary to bulk carriers, for which le ~ Ltr is given by the disorder correlation length ξ (isotropic scattering due to a short-range disorder potential), the transport length of both upper and lower topological surface states was found to be much larger than the mean-free path, despite a limitation at about 200 nm probably due to the finite coupling with bulk carriers [larger values are expected for decoupled topological states and/or in materials with a larger disorder correlation length, such as Bi2Te3].
The average number of scattering centers involved in a backscattering process is directly related to the ratio Ltr/le, and it can give some important information on the nature of both the scattering potential and the quasi-particles. Importantly, we revealed the long-range nature of disorder for spin-helical surface Dirac fermions, due to efficient electrostatic screening and spin-momentum locking, which results in strongly anisotropic scattering, as observed by local probe microscopy. This means that forward scattering is favored for such quasi-particles and that the transport length is strongly enhanced (Ltr >> le), as predicted by theory [8] and confirmed by trans-conductance measurements [17]. Such a situation never happens in other materials within which charge carriers directly coexist with disorder (including Dirac fermions in graphene), where the scattering of quasi-particles by any kind of disorder is isotropic (that is, Ltr ~ le). Only high-mobility AlGaAs 2DEGs can realize such a situation of anisotropic scattering. In this case, however, this is due to the spatial separation of free carriers and localized ionized donors, and it is not possible to vary the degree of disorder over a wide range, so that there is little room to investigate quasi-ballistic transport (in other words, the transition from ballistic to diffusive transport is rather abrupt and happens already when a small amount of impurities are introduced in the system). This is not the case for spin-helical Dirac fermions, and this property is at the origin of their unique transport properties, particularly in nanostructures, with an extended range of parameters to study quasi-ballistic transport, and therefore the ballistic-to-diffusive crossover in mesoscopic conductors.
This enhanced transport length for topological surface states is also important for spin transport studies, as it gives a lower limit for the size of functional spintronic devices making use of the spin-momentum locking property. Indeed, due to the strong spin-orbit coupling, there is a direct correspondence between the momentum-backscattering transport length and the spin relaxation length. With wide Bi2Se3 nanostructures, this scale is rather short (~200 nm), [17] so that, for instance, lateral spin valves could only be realized in the short-junction limit. This also shows that the true potential for the spin-to-charge conversion in highly-disordered Bi2Se3 could still give an improvement in the conversion efficiency by two orders of magnitude with respect to state-of-the-art records, with an inverse Edelstein length lIEE determined by the intrinsic transport length of the 3D topological insulator, whereas it presently remains limited by the spin/momentum relaxation below metallic ohmic contacts (with lIEE ~ 2 nm).
2.4. Dimensionalities of transport
The enhancement of the transport length for topological surface states also has two fundamental consequences for the quantum transport properties of 3D TI nanostructures and the dimensionality of surface charge transport:
The phase coherence length of TSS is also enhanced in the same ratio for diffusive 2D surface states in nanoplatelets or wide nanoribbons, so that mesoscopic transport can be studied in rather wide and long conductors (well beyond the micron size), despite relatively strong disorder. Since Lϕ >> Ltr (Lϕ being determined by inelastic scattering), quantum corrections to the conductance due to diffusive phase-coherent transport can thus be revealed by magneto-transport measurements with magnetic fields as small as 100 mT.
The condition for ballistic transport in the transverse motion of surface carriers along the perimeter is more restrictive (Lp < 2 Ltr), but it can be fulfilled for rather long (Lp ~ 500 nm), and therefore with nanostructures having a large cross section (S ~ 0.2 μm2). Contrary to the case of carbon nanotubes, magnetic flux-dependent periodic phenomena in these quantum wires (such as the Aharonov-Bohm interference) can therefore be studied in rather small fields, below 1 T.
In the case of highly-disordered Bi2Se3 nanostructures (le ~ 30 nm), large values of Ltr (>200 nm) [17] and of Lφ (>2 μm) [39] were found. This implies that the dimensionality of surface-state transport is reduced in narrow nanostructures (mostly nanowires) and that their band structure is modified due to quantum confinement (which even further reduces the scattering by disorder). It thus becomes important to distinguish between three different situations for the dimensionality of charge transport:
No quantum confinement [Ltr is shorter than every dimensions]. Surface-state transport is diffusive and quasi-particles are 2D spin-helical Dirac fermions with a continuous spin-helical Dirac-cone band structure.
Transverse quantum confinement [the perimeter Lp becomes shorter than 2 Ltr]. Surface-transport is quasi-ballistic if the distance between contacts is longer than Ltr and ballistic otherwise. The length L remains much larger than Ltr, so that surface modes are quasi-1D channels in such long nanowires (becoming truly 1D only when they close).
Full quantum confinement [all dimensions are shorter than Ltr]. Spin-helical Dirac fermions are then fully localized in a short nanowire, which becomes a 0D quantum dot.
We remark that the dimensionality of quantum coherent transport is another quantity determined by comparing the dimensions of a mesoscopic conductor to the phase coherent length Lφ. Since Lφ is longer than Ltr, nanoribbons with a width W, such as Ltr < W < Lφ, have 2D spin-helical surface Dirac fermions but quantum coherent transport is 1D (which modifies the self-averaging of quantum interference in long conductors, for which the length L is longer than Lφ).
3. Transport properties of quasi-1D topological surface states
Signatures of the quasi-ballistic transport of topological surface states in 3D TI quantum wires can be revealed by the study of quantum corrections to the conductance. In a bulky nanostructure, spin-helical Dirac fermions propagate on the surface in a hollow-type electrical geometry, in analogy to carbon nanotubes (ballistic transport) or to the Sharvin-Sharvin metallic tubes (diffusive transport). Phase-coherent transport in the transverse direction (along the perimeter of the nanowire) thus gives rise to periodic Aharonov-Bohm oscillations in the longitudinal magneto-conductance, determined by a well-defined cross section S = LP2/(4\\ϕ), and their observation in wide Bi2Te3 nanoribbons gave the first robust evidence of surface states by transport measurements [40]. Their topological nature was then confirmed by a study of decoherence at very low temperatures in narrow (quantum) nanowires [39], which revealed the unusual weak coupling to the environment and the ballistic motion in the transverse direction. Later, phase-coherent transport in the longitudinal direction was investigated in a study of conductance fluctuations [18], which revealed the subtle influence of disorder in the quasi-ballistic regime, leading to a non-universal behavior of quantum interference. A detailed understanding of the propagation of spin-helical 1D surface modes showed that both the spin texture of Dirac fermions and their quantum confinement are responsible for the weak scattering by disorder [41], thus leading to the weak coupling between quantum states, a necessary condition for their manipulation by radio-frequency fields, as well as for the study of specific properties related to a single topologically-protected low-energy mode, such as 1D chiral edge states or Majorana bound states [42].
3.1. Quantum confinement: 1D Dirac spectrum
In quantum wires (Lp < 2 Ltr), the surface-state band structure is modified by periodic boundary conditions imposed in the transverse direction of the nanostructure, leading to the quantization of the transverse momentum k⊥ (Figure 5b). This situation is equivalent to the energy quantization of quasi-particles confined into a quantum well with infinitely-high potential barriers, and for Dirac fermions, the transverse energy becomes quantized with a constant energy-level spacing Δ = hvF 1/Lp between successive transverse modes. Due to the winding of the wave function along the perimeter (curvature) and to the spin-momentum locking of helical Dirac fermions, an additional Π Berry phase suppresses the topological protection of all energy modes in zero magnetic field (pairs of gapped states). However, if a magnetic field is applied along the nanowire axis, the Aharonov-Bohm flux modifies the periodic boundary condition (which gives an overall shift of transverse quantization planes, thus tuning the energy spectrum). Importantly, this flux dependence can restore the topological protection periodically when the Aharonov-Bohm phase compensates the curvature-induced Berry phase, giving rise to a single gapless and linear mode with perfect transmission (Figure 5c), independent of disorder [43].
Figure 5.
(a) Scanning electron microscope image of a narrow Bi2Se3 nanowire, with a perimeter Lp = 300 nm. Dashed lines separate different facets. Inset: schematics of the cross section and coherent winding of topological surface states; (b) transverse-impulse quantization planes intersecting the spin-helical Dirac cone. By applying a magnetic flux, all planes are continuously shifted in the k⊥ direction; (c) resulting band structures for two different values of the magnetic flux ϕ. For ϕ = 0, quantum confinement gives pairs of modes with a finite energy gap Δ. For ϕ = 1/2ϕ0, a single topological mode with linear dispersion appears (quantization plane intersecting the Dirac point); (d) energy broadening Γ of the quantized transverse energy due to disorder [for 3DTI quantum wires, Γ is smaller than Δ, even for relatively strong disorder].
In recent years, a couple of interesting studies suggested the influence of such a topological mode on quantum transport properties, particularly the Aharonov-Bohm (AB) oscillations [32, 33, 44]. These results raised some important questions since it was not possible to give a quantitative interpretation of the physical phenomena observed (Aharonov-Bohm oscillations and non-universal conductance fluctuations) solely based on the contribution of this perfectly transmitted mode to the conductance. In particular, the amplitude of these quantum corrections to the conductance was always found much smaller than the conductance quantum G0. It thus remained unclear whether these properties were a signature of a topological transition or were rather induced by all spin-textured modes, including dominant contributions from high-energy quasi-1D modes. Actually, the quantum magneto-conductance is mostly due to a limited number of modes, those partially-opened modes with a quantized transverse energy close to the Fermi energy. Since most studies were conducted in the large-N limit (EF >> Δ), the relative contribution of the topological surface mode is therefore rather small. A full quantitative understanding required to describe the energy dependence of the transmissions for all surface modes, considering both disorder and interfaces with metallic contacts (see Section 3.4 for details). In particular, the scattering of surface modes by disorder results in the energy broadening Γ of quantized modes (Figure 5d). We evidenced that the quasi-ballistic regime is closely related to the condition Γ << Δ, which is satisfied over an unusual broad parameters range (disorder strength, energy) in 3D topological insulator nanostructures [41].
The quantum coherent transport of topological surface states in the transverse direction of a 3D TI nanostructure results in conductance oscillations when a longitudinal magnetic induction B// is applied (hence a magnetic flux ϕ = B//*Sel, where Sel is the effective electrical cross section of metallic surface states). This is due to the flux-periodic evolution of the Aharonov-Bohm quantum interference giving successive conductance maxima (constructive interference) and minima (destructive interference). Because the phase coherence length can be as large as a couple of micrometers (at very low temperatures), two different situations must be considered for coherent transport in the transverse motion of surface states:
When Lϕ ~ Lp/2, clear periodic oscillations of the conductance are directly visible in the longitudinal magneto-conductance G(B//). In this case (wide nanoribbons), only the fundamental-harmonic Aharonov-Bohm interference modifies the conductance, a behavior which already reveals that the phase averaging due to disorder is not efficient, despite a high point-defect density in most 3DTI materials.
When Lϕ >> Lp, that is, either at very low temperatures or for short-perimeter nanowires (quantum wires), the periodic AB behavior is usually hidden in complex G(B//) traces. This is due to the multiple-harmonic contributions to the transverse quantum interference (related to the multiple winding of coherent trajectories along the perimeter), and to the influence of disorder (phase shifts). The periodic behavior can, however, be revealed by a Fourier transform analysis.
3.2.1. Case of wide nanoribbons (long-perimeter limit, with Lϕ ~ Lp/2)
For wide nanoribbons, periodic Aharonov-Bohm oscillations are directly visible in G(B//) traces, with a rather small amplitude typical for the large-N limit in a mesoscopic conductor, where N is the number of populated transverse modes, with N = EF/2Δ, since Δ = hvF/Lp is smaller than E_F). As seen in Figure 6 for a wide Bi2Te3 nanoribbon (EF ~ 120 meV; Lp = 940 nm; Δ = 2 meV), the Aharonov-Bohm period, δBAB = 150 mT, directly relates to the electrical cross section of the nanostructure, with a value being slightly smaller than that given by its physical dimensions (the topological surface states being “burried” below a thin native oxide layer, typically 5 nm thick). The fast-Fourier transform of the G(B//) trace thus gives a single peak at the AB frequency.
Figure 6.
(a) Scanning electron microscope image of a Bi2Te3 nanowire with a rather large perimeter Lp = 940 nm (width w = 400 nm, height h = 70 nm) and ohmic CrAu contacts; (b) Aharonov-Bohm periodic oscillations (fundamental harmonics), with a period δB_AB that directly relates to the nanowire’s cross section. After [18].
According to theory, the overall phase shift of this sine evolution due to the AB quantum interference depends on both the degree of disorder and the energy of Dirac quasi-particles [43]. In most cases, the Fermi energy is very large and AB oscillations are phase locked with a conductance maximum in zero magnetic field, as found in many experiments and confirmed by theory. Yet, theory predicts the opposite situation (conductance minimum for a zero magnetic flux) when the chemical potential is near the Dirac point. The overall energy dependence of this phase shift can be quantitatively obtained from models taking explicitly disorder into account, and it allowed us to reveal an oscillatory behavior that is directly related to quantum confinement (see Section 3.4).
For lower temperatures (longer Lφ) or for narrower nanoribbons, roughly when Lφ ~ Lp, additional Altshuler-Aronov-Spivak (AAS) oscillations develop in addition. These correspond to quantum interference related to the complete winding of coherent paths along the perimeter, with time-reversed coherent loops so that this contribution is never damped by disorder, which is the usual situation found in (diffusive) mesoscopic conductors.
3.2.2. Case of narrow (quantum) nanowires (short-perimeter limit, Lp < 2 Ltr << Lφ)
For narrow nanostructures, the conductance modulation due to both AB and AAS interferences results from a complex mixing of high-order harmonics (multiple windings of coherent loops), with harmonic-dependent phase shifts induced by disorder and varying relative amplitudes due to quasi-ballistic transport. The periodic-flux dependence of the longitudinal magneto-conductance is therefore hardly visible in most G(B//) traces, though it can still be when low-order harmonics remain dominant (as shown in Figure 7b). Since this periodic behavior is specific to topological surface states (with a flux-periodic energy spectrum), it can always be unveiled by a careful fast-Fourier transform analysis, provided that enough oscillations are measured (that is, when the field range largely exceeds the fundamental AB period). For a micron-long Bi2Se3 quantum wire with perimeter Lp = 280 nm, up to six harmonics were clearly resolved at very low temperature, as seen in Figure 7c) [39].
Figure 7.
(a) Scanning electron microscope image of a narrow Bi2Se3 nanowire with a rather short perimeter Lp = 280 nm and ohmic Al contacts; (b) Aharonov-Bohm periodic oscillations, with the first two harmonics directly visible in the G(B//) trace; (c) fast-Fourier transform revealing higher-order harmonics, up to n = 6 at very low temperature. After [39].
For short wires (L ~ LφBS), we also remark that a complication comes further from that aperiodic conductance fluctuations due to bulk carriers coexist with surface periodic AB oscillations [although LφBS < LφSS, the self-averaging of coherent bulk transport is reduced at very low temperatures due to their charge transport dimensionality d = 3 and to longer LφBS values]. Besides, because G(B//) curves are measured over a finite field range, the FFT of bulk aperiodic conductance fluctuations often results in a non-monotonous background, possibly giving “peaks” but with no relation to a periodic behavior, contrary to that of G(B//) changes due to the AB interference.
The ballistic nature of the transverse motion in such quantum wires results in an unusual temperature dependence of the phase coherence length LφSS, with a 1/T behavior observed for all harmonics. This is the signature of both ballistic transport (Lφ = vFτφ) and a decoherence time τφ ~ 1/T limited by a weak coupling to fluctuations of the environment [39]. All other scenarios based on decoherence limited by either the Nyquist noise or the thermal noise give a very different power-law dependence.
An extra signature of the quasi-ballistic regime is also found when considering the relative amplitude of AB harmonics. Contrary to the case of a diffusive mesoscopic conductors, their amplitudes are not increasingly small for higher orders n and they cannot be described by an exponential damping behavior related to the ratio Lφ/Ln, where Ln = n*Lp [39]. This is due to disorder and to both geometric and contact effects, which all influence details of the quantum interference for different quantum coherent paths, in the quasi-ballistic regime [41]. In general, it thus remains difficult to investigate details of the AB oscillations in this regime, due to the complex mixing of all harmonics in the presence of disorder, which varies for different configurations of the microscopic disorder (as obtained by thermal cycling at room temperature of a given mesoscopic conductor).
More information about the weak scattering of quantized surface modes by a non-magnetic disorder can be obtained by studying the (static) conductance fluctuations due to the longitudinal motion of surface carriers in a highly-disordered 3DTI quantum wire. Contrary to the case of a diffusive mesoscopic conductor, their statistical properties such as the conductance variance are not universal and they can vary when the quantized Dirac band structure is modified by an Aharonov-Bohm flux [18]. Using a 3D vector magnet, we could vary independently the longitudinal field (tuning of the energy spectrum; transverse motion) and the transverse magnetic field (probing the aperiodic conductance fluctuations due to disorder; longitudinal motion). This provides the complete mapping of quantum interference, as seen in Figure 8a). It was shown that the absolute amplitude of the conductance variance varG = δGrms2 = <G-<G>>2 has a periodic modulation with the magnetic flux (Figure 8b), a property specific to surface transport (well-defined cross section). This behavior is well captured by numerical calculations (Figure 8c and d), which also reproduce the correct amplitude of this modulation mod(varG). We evidenced that non-universal conductance fluctuations are the signature of the weak coupling between transverse quantized modes induced by disorder, and we inferred the amplitude of the disorder broadening Γ from the temperature dependence of the modulation mod(VarG), in rather good agreement with numerical calculations [18]. Because Γ << Δ, quasi-ballistic transport is a common property to all populated surface modes, each of them giving a significant contribution to the conductance (close to G0) as compared to that of the perfect transmission case (G0). Besides, the sharp evolution of varG with the energy of successive transverse modes (Figure 8c) suggested that only a limited number of partially-opened modes (nearby EF) contribute to the conductance fluctuations, due to a rapid energy dependence of the transmission for all channels.
Figure 8.
(a) Quantum corrections to the conductance of a Bi2Se3 quantum wire mapped over a large range of longitudinal magnetic fields (magnetic flux) and transverse magnetic fields, at very low temperature; (b) flux-dependence of the conductance variance revealing a non-universal behavior and a periodic evolution, a signature of the quasi-ballistic transport of Dirac surface modes; (c and d) numerical calculations of the energy (c) and flux (d) dependences of the conductance variance in a disordered 3DTI quantum wire, showing periodic evolutions due to quantum confinement of all transverse modes. After [18].
3.4. Quasi-ballistic transport: disorder and transmissions
To evidence that this interpretation is actually very general to all quantum corrections to the conductance in 3DTI quantum wires, it is important to calculate the energy dependence of the transmissions for all modes, taking disorder into account but also interfaces with metallic contacts. This was done in a comparative study of numerical calculations with an analytical model that captures the main property common to all quasi-1D spin-helical surface modes, that is, the suppression of scattering due to quantum confinement [41]. The set of transmissions Ti represents the mesoscopic code of a coherent conductor, from which all important quantities can be calculated [45], the simplest one being the total conductance G = ∑TiG0. Importantly, the transmissions were found to nearly reach unity for all modes when their longitudinal kinetic energy exceeds Δ (Figure 9). The same (rapid) evolution was found even for high-energy modes, though over a slightly broader energy window, thus explaining why quasi-ballistic transport properties exist for many modes over a broad energy range. This also shows that diffusive longitudinal transport is realized only for conductor lengths that largely exceed the transport length. Contrary to the case of 2D quasi-particles with isotropic scattering for which the transition from the ballistic to the diffusive regime is rather abrupt (le < L < Ltr, with Ltr ≤ 2 le), the quasi-ballistic regime in 3DTI quantum wires exists over a wider parameter range (Ltr/2 < L < α Ltr, with Ltr >> le and α is related to the aspect ratio L/Lp). This unusual behavior, related to the enhanced transport length, is due to both the spin texture of Dirac modes (anisotropic scattering) and to their large confinement energy in quantum wires, both favoring the weak scattering of quantized modes by disorder.
Figure 9.
Energy dependence of the surface-mode transmissions in disordered 3D topological insulator quantum wires, for three values of the disorder strength g=0.02 (a), g=0.2 (b), and g=1 (c). After [41].
3.4.1. Scattering by disorder and contacts
Considering the scattering by disorder as due to a random potential of energy barriers (Gaussian disorder, with a correlation length ξ, see Figure 10a), it is possible to give an analytical description of the transmissions of high-energy modes propagating between two transparent ohmic contacts, for different degrees of disorder from the clean limit (ballistic, Fabry-Pérot) to the dirty limit (diffusive) [41]. In the quasi-ballistic regime, we found that the conductance is determined by the interfaces with metallic contacts (similarly to a clean conductor) and not by details of the microscopic disorder in the quantum wire. Due to the quantum confinement of Dirac fermions with evenly-spaced energy levels, the energy dependence of the conductance can oscillate at low energies (whereas its has a linear dependence at high energy, as for the 2D limit) and the average transmission per mode only depends on the nature of the contacts. For an intermediate disorder strength g, Fabry-Pérot interferences are suppressed by efficient phase averaging, and inter-mode scattering results in an oscillatory energy dependence of the transmission, due to the increased density of states at the onset of a nearby mode and because disorder broadening remains smaller than the energy level spacing. This can be directly seen in the energy dependence of the transmission of a high-energy mode in a Bi2Se3 quantum wire (using a realistic value of ξ), as shown in Figure 10b). For very large values of g, Γ exceeds Δ and charge transport becomes diffusive.
Figure 10.
(a) Quantized band structure of surface modes for a magnetic flux ϕ = 1/2ϕ0 and inter-mode scattering induced by a random disorder potential δV; (b) energy dependence of the transmission of the m = 9 quantized mode for ϕ = 0, showing resonances due to disorder-induced inter-mode mixing, with an energy broadening Γ. After [41].
To understand why the quasi-ballistic regime exists over a broad range of parameters, it is important to consider the energy dependence of the transport length [see [41] for details], as shown in Figure 11 for different g values. Contrary to the case of massive quasi-particles, Ltr does not vanish at low energy for Dirac fermions in 1D. Instead, it diverges and a similar behavior occurs at high energy, due to the anisotropy of scattering. As a consequence, the transport length has a minimum value that depends on the strength of disorder. For a given disorder correlation length ξ, this minimum value is obtained for kξ ≈ 1 and the values of Ltrmin can be much larger than the transverse dimensions of the nanostructure for all energies, for a broad range of g values, so that the condition for quasi-ballistic transport is always fulfilled for such highly-disordered 3D topological insulator quantum wires. Good agreement was found between this simplified analytical model and numerical calculations, for that details of the microscopic disorder do not affect the conductance in this regime, which is mostly determined by metallic contacts.
Figure 11.
Energy dependence of the transport length l in a quantum wire with a perimeter W = Lp and a transverse energy quantization Δ is calculated for three different strengths of the disorder potential. Red dotted lines show asymptotic behaviors related to the divergence of l = Ltr at low or high energies, due to the density of states or to the anisotropy of scattering, respectively. In all cases, the transport of all surface modes is ballistic or quasi-ballistic. After [41].
3.4.2. Quantitative derivation of the Aharonov-Bohm amplitude
Based on the transmissions calculated for different values of the magnetic flux (corresponding to different quantized energy spectra), it is possible to calculate the energy dependence of Aharonov-Bohm oscillations. As seen in Figure 11, their amplitude decreases with the energy of surface modes and a good quantitative agreement with experiments are found at high energies. The oscillatory behavior reported in experiments is also well reproduced, as well as energy-periodic phase shifts [33] which are actually due to the quantized band structure (Figure 12) [41].
Figure 12.
(a) Energy dependence of the Aharonov-Bohm amplitude, rapidly decreasing from the conductance quantum G0 (contribution of the topological mode only) to a fraction of G0 (contribution of higher-energy transverse modes); (b) flux dependence of the conductance for different energies, from 0 to 4.5 Δ (successive thin lines correspond to an energy change 0.05 Δ and thick lines to multiple values of 1/2 Δ). Phase shifts are due to the quantized energy spectrum of surface modes. The influence of the topological mode is seen only for very low energies. After [41].
3.4.3. Perfectly-transmitted topological mode
To evidence the influence of the topological mode on the conductance, it is therefore necessary to set the mesoscopic conductor in specific conditions:
In long wires, the transmission of all modes but the topological one should be reduced. However, the spin texture of surface Dirac states prevents the strong localization of high-energy modes, so that this is not a good strategy for highly-doped quantum wires (as this is the case for Bi2Se3 nanostructures).
In the small-N limit (less than about 4–5 modes populated), the relative influence of the topological mode on the quantum magneto-conductance will be larger, also in short wires. This condition is rather restrictive and requires either to bring the electro-chemical potential close to the Dirac point or to achieve very large values of Δ.
With the goal to investigate the physics of 3D TI quantum wires close to the Dirac point, best results could be obtained in long and ultra-narrow nanostructures [46, 47], since low-energy modes other than the topological mode have a reduced transmission due to disorder (minimum of the backscattering length, so that Ltr << L and G<<G0). Furthermore, since the transport of surface modes is quasi-ballistic, it will become important to optimize/control the coupling between metallic contacts and the transverse wave function of a given mode. In particular, the amplitude of probability can have an azimuthal angle dependence, which varies from one mode to another, so that quantum transport properties will ultimately depend on the exact geometry of the mesoscopic conductor. Also, the low-energy spectrum can be modified by a large transverse magnetic field. For a rectangular cross section (Figure 13), a striking property is related to the evolution of the topological mode from a helical state to a chiral edge state, when a moderate transverse magnetic field is applied [42]. The specific orbital response of such 3DTI quantum wires correponds to an intermediate situation between the quantum spin Hall in a 2D TI and the Quantum Hall effect in 2DEGs.
Figure 13.
Energy spectrum of a 3DTI quantum wire with a rectangular cross section (h = 40 nm; w = 160 nm) for η = ϕ/ϕ0 = 0 (left) and η = ϕ/ϕ0 = ½ (center; right), low-energy band structure in the presence of a large transverse magnetic induction B⊥ = 2 T, showing the emergence of chiral edge states without dispersion over a wide range of impulse, independent of η. After [42].
The control of low-energy quantum states in 3DTI nanostructures would offer novel opportunities for their quantum manipulation as well as for spin filtering, tuning the quantum states with an electric or a magnetic field. When coupled to metallic electrodes with gapped excitations, the topological mode generates novel quantum states with an intrinsic topological protection, such as Majorana bound states or spin-polarized edge states in the quantum anomalous Hall regime. These could be important for quantum dynamics studies, with limited decoherence. Non-topological low-energy modes are also interesting for their energy tuning, by a gate voltage or a magnetic flux, which is associated with a continuous change of their spin state between nearly-orthogonal states. Besides, these can be either 1D extended states (long quantum wires) or 0D localized states (short quantum wires, that is, for L < Ltr).
4. Conclusion and perspectives
The weak coupling of surface states in 3D topological insulator quantum wires, due to both their spin texture and the quantum confinement of Dirac fermions, gives unique opportunities to control novel quantum states in mesoscopic conductors, despite non-magnetic disorder. Yet, it remains difficult to control a small number of transverse quantized states close to the Dirac degeneracy point, mostly due to intrinsic limitations in conventional 3DTIs materials. Whereas the Bi2Se3 family offers many advantages (tunable band structure in solid solutions of ternary compounds and high-quality single-crystalline nanostructures), it remains difficult to achieve surface transport only, and, most important, to control low-energy surface quasi-particles (large residual bulk doping or interface charge transfer, due to disorder).
Therefore, the next generation of electronic devices based on 3D topological insulators will necessarily be developed from advanced functional nanostructures and heterostructures. One of the most important challenge will be the full control of interface band bending, with a high-enough interface quality so as to optimize the coupling between metallic contacts and spin-helical surface Dirac fermions. For instance, this is particularly true for spin transport experiments, which require to minimize the momentum/spin relaxation below the contacts in order to make use of the intrinsic potential of electronic states with spin-momentum locking.
Toward this goal, new growth and nanofabrication methods need to be envisioned, in combination with those already used to prepare high-quality single-crystalline nanostructures (vapor transport, vapor-liquid-solid epitaxy, and chemical-vapor deposition). Novel techniques, such as the in-situ stencil lithography of metallic contacts combined the growth of ultra-thin films by molecular beam epitaxy, already gave some promising results, for instance to realize highly-transparent superconducting contacts and investigate topological superconductivity [48]. Also, atomic layer epitaxy holds promises to realize core-shell lateral nanostructures adapted to the control of the electro-chemical potential at the interface with a topological insulator [49, 50, 51].
Acknowledgments
This work was supported by the German Research Foundation DFG through the SPP 1666 Topological Insulators program. This book chapter reviews our previous work on 3D topological insulator quantum wires, for which we acknowledge the contributions of our collaborators: J. H. Bardarson, B. Büchner, J. Cayssol, B. Dassonneville, B. Eichler, W. Escoffier, H. Funke, S. Hampel, C. Nowka, O.G. Schmidt, J. Schumann, L. Veyrat, K. Wruck, and E. Xypakis.
Conflict of interest
The authors declare no conflict of interest.
\n',keywords:"3D topological insulators, nanostructures, quantum confinement, Dirac fermions, spin transport, disorder, core-shell heterostructures",chapterPDFUrl:"https://cdn.intechopen.com/pdfs/62233.pdf",chapterXML:"https://mts.intechopen.com/source/xml/62233.xml",downloadPdfUrl:"/chapter/pdf-download/62233",previewPdfUrl:"/chapter/pdf-preview/62233",totalDownloads:659,totalViews:233,totalCrossrefCites:0,totalDimensionsCites:0,hasAltmetrics:1,dateSubmitted:"October 18th 2017",dateReviewed:"March 2nd 2018",datePrePublished:null,datePublished:"July 25th 2018",dateFinished:null,readingETA:"0",abstract:"The next generation of electronic devices based on 3D topological insulators will be developed from advanced functional nanostructures and heterostructures. Toward this goal, single-crystalline nanowires offer interesting opportunities for new developments due to the strong quantum confinement of spin-helical surface Dirac fermions and to the possibility to realize core-shell lateral nanostructures adapted to the control of the electro-chemical potential at the interface with a topological insulator. Here, we review the specific transport properties of 3D topological insulator quantum wires and the influence of disorder. Having a large energy quantization, weakly-coupled Dirac surface modes are prone to quasi-ballistic transport, with some analogies to carbon nanotubes but with spin-textured quantum states weakly coupled by non-magnetic disorder. Due to a small interaction with their environment, these surface modes are good candidates to realize novel quantum spintronic devices, spanning from ballistic spin conductors to localized spin filters. A specific topological mode also holds promises to control chiral edge states and Majorana bound states in truly 1D quantum wires, being tunable with a magnetic field or an electrical gate. Challenges toward these goals are briefly discussed, as well as the need for novel functional heterostructures.",reviewType:"peer-reviewed",bibtexUrl:"/chapter/bibtex/62233",risUrl:"/chapter/ris/62233",book:{slug:"heterojunctions-and-nanostructures"},signatures:"Romain Giraud and Joseph Dufouleur",authors:[{id:"228460",title:"Dr.",name:"Romain",middleName:null,surname:"Giraud",fullName:"Romain Giraud",slug:"romain-giraud",email:"romain.giraud@cea.fr",position:null,institution:null},{id:"228464",title:"Dr.",name:"Joseph",middleName:null,surname:"Dufouleur",fullName:"Joseph Dufouleur",slug:"joseph-dufouleur",email:"j.dufouleur@ifw-dresden.de",position:null,institution:null}],sections:[{id:"sec_1",title:"1. Introduction",level:"1"},{id:"sec_2",title:"2. Transport properties of 2D topological surface states",level:"1"},{id:"sec_2_2",title:"2.1. Nanostructures of 3D topological insulators for surface-transport studies",level:"2"},{id:"sec_3_2",title:"2.2. Band bending and interface charge transfers",level:"2"},{id:"sec_4_2",title:"2.3. Anisotropic scattering and charge transport length (=spin diffusion length)",level:"2"},{id:"sec_5_2",title:"2.4. Dimensionalities of transport",level:"2"},{id:"sec_7",title:"3. Transport properties of quasi-1D topological surface states",level:"1"},{id:"sec_7_2",title:"3.1. Quantum confinement: 1D Dirac spectrum",level:"2"},{id:"sec_8_2",title:"3.2. Quantum coherence I: Aharonov-Bohm oscillations",level:"2"},{id:"sec_8_3",title:"3.2.1. Case of wide nanoribbons (long-perimeter limit, with Lϕ ~ Lp/2)",level:"3"},{id:"sec_9_3",title:"3.2.2. Case of narrow (quantum) nanowires (short-perimeter limit, Lp < 2 Ltr << Lφ)",level:"3"},{id:"sec_11_2",title:"3.3. Quantum coherence II: non-universal conductance fluctuations",level:"2"},{id:"sec_12_2",title:"3.4. Quasi-ballistic transport: disorder and transmissions",level:"2"},{id:"sec_12_3",title:"3.4.1. Scattering by disorder and contacts",level:"3"},{id:"sec_13_3",title:"3.4.2. Quantitative derivation of the Aharonov-Bohm amplitude",level:"3"},{id:"sec_14_3",title:"3.4.3. Perfectly-transmitted topological mode",level:"3"},{id:"sec_17",title:"4. Conclusion and perspectives",level:"1"},{id:"sec_18",title:"Acknowledgments",level:"1"},{id:"sec_21",title:"Conflict of interest",level:"1"}],chapterReferences:[{id:"B1",body:'Hasan MZ, Kane CL. Topological insulators. Reviews of Modern Physics. 2010;82:3045'},{id:"B2",body:'Qi X-L, Zhang S-C. Topological insulators and superconductors. Reviews of Modern Physics. 2011;83:1057'},{id:"B3",body:'Bernevig BA, Zhang S-C. Quantum spin Hall effect. Physical Review Letters. 2006;96:106802'},{id:"B4",body:'Kane CL, Mele EJ. 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Univ. Grenoble Alpes, CNRS, CEA, Grenoble-INP, Institute of Engineering Univ. Grenoble Alpes, INAC-Spintec, France
Leibniz Institute for Solid State and Materials Research, IFW Dresden, Germany
Leibniz Institute for Solid State and Materials Research, IFW Dresden, Germany
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May,\nKannaiyan Pandian and Oluwatobi S. Oluwafemi",authors:[{id:"99092",title:"Prof.",name:"Samuel Oluwatobi",middleName:null,surname:"Oluwafemi",fullName:"Samuel Oluwatobi Oluwafemi",slug:"samuel-oluwatobi-oluwafemi"},{id:"188914",title:"Dr.",name:"K",middleName:null,surname:"Pandian",fullName:"K Pandian",slug:"k-pandian"},{id:"208652",title:"Dr.",name:"Sundararajan",middleName:null,surname:"Parani",fullName:"Sundararajan Parani",slug:"sundararajan-parani"},{id:"208653",title:"Mrs.",name:"Ncediwe",middleName:null,surname:"Tsolekile",fullName:"Ncediwe Tsolekile",slug:"ncediwe-tsolekile"},{id:"208654",title:"Ms.",name:"Bambesiwe",middleName:null,surname:"May",fullName:"Bambesiwe May",slug:"bambesiwe-may"}]},{id:"56933",title:"Quantum Dots and Fluorescent and Magnetic Nanocomposites: Recent Investigations and Applications in Biology and Medicine",slug:"quantum-dots-and-fluorescent-and-magnetic-nanocomposites-recent-investigations-and-applications-in-b",signatures:"Anca Armăşelu",authors:[{id:"189080",title:"Dr.",name:"Anca",middleName:null,surname:"Armăşelu",fullName:"Anca Armăşelu",slug:"anca-armaselu"}]}]}]},onlineFirst:{chapter:{type:"chapter",id:"65626",title:"Nematicity in Electron-Doped Iron-Pnictide Superconductors",doi:"10.5772/intechopen.84408",slug:"nematicity-in-electron-doped-iron-pnictide-superconductors",body:'
1. Introduction
The discovery of Fe-based superconductors with critical temperatures up to 55 K has begun a new era of investigations of the unconventional superconductivity. In common with copper-like superconductors (cuprate), the emergency of superconductivity in electron-doped Fe-pnictides such as BaFe1−xCoxAs2 is to suppress the magnetic order and fluctuations originated in the parent compound with x=0 [1]. The intertwined phases between the superconductivity and stripe spin density wave (SDW) order (ferromagnetic stripes along one Fe-Fe bond direction that is antiferromagnetically aligned along orthogonal Fe▬Fe bond) are of particular interests. In both pnictides and cuprates, the experimentally observed nematicity exists in an exotic phase between the superconductivity (SC) and the stripe SDW [2]. The nematicity occurs in weakly doped iron pnictides with tetragonal-to-orthorhombic structural transition [3, 4, 5, 6, 7, 8, 9, 10, 11, 12, 13, 14, 15, 16, 17], i.e., in a square unit cell, the point-group symmetry is reduced from C4 (tetragonal) to C2 (orthorhombic).
At present, there are two scenarios for the development of nematic order through the electronic configurations [18]. One scenario is the orbital fluctuations [19, 20, 21, 22, 23]. The structural order is driven by orbital ordering. The orbital ordering induces magnetic anisotropy and triggers the magnetic transition at a lower temperature. The other scenario is the spin fluctuation [24, 25, 26, 27]. The magnetic mechanism for the structural order is associated with the onset of SDW.
Recently, Lu et al. [28] reported that the low-energy spin fluctuation excitations in underdoped sample BaFe1.915Ni0.085As2 change from C4 symmetry to C2 symmetry in the nematic state. Zhang et al. [29] exhibited that the reduction of the spin-spin correlation length at 0π in BaFe1.935Ni0.065As2 happens just below Ts, suggesting the strong effect of nematic order on low-energy spin fluctuations. Apparently, these experiments above have provided a spin-driven nematicity picture.
The partial melting of SDW has been proposed as the mechanism to explain the nematicity. The properties of the spin-driven nematic order have been studied in Landau-Ginzburg-Wilson’s theory [18, 24, 25, 26]. Meanwhile, the lack of the realistic microscopic model is responsible for the debates where the leading electronic instability, i.e., the onset of SDW, causes the nematic order. Recently, an extended random phase approximation (RPA) approach in a five-orbital Hubbard model including Hund’s rule interaction has shown that the leading instability is the SDW-driven nematic phase [30]. Although the establishment of the nematicity in the normal state has attracted a lot of attentions, the microscopic description of the nematic order and, particularly, the relation between SC and the nematic order are still missing.
The magnetic mechanism for the structural order is usually referred to the Ising-nematic phase where stripe SDW order can be along the x-axis or the y-axis. The nematic phase is characterized by an underlying electronic order that the Z2 symmetry between the x- and y- directions is broken above and the O(3) spin-rotational symmetry is preserved [25].
The magnetic configuration in FeSCs can be described in terms of two magnetic order parameters ∆x and ∆y. Both order parameters conventionally defined in momentum space are written as
∆ℓ=∑kck+Qℓ,α†σαβck,β,E1
where ℓ=x or y. Here the wave vectors Qx=π0 and Qy=0π correspond to the spins parallel along the y-axis and antiparallel along the x-axis and the spins parallel along the x-axis and antiparallel along the y-axis, respectively.
In the stripe SDW state, the order parameters are set to ∆x≠0 or ∆y≠0, i.e., ∆ℓ≠0. This implies to choose an ordering vector either Qx or Qy. The Z2 symmetry indicating to the degenerate of spin stripes along the y-axis (corresponding to Qx) or x-axis (corresponding to Qy) is broken. In addition, the O(3) spin-rotational symmetry is also broken. In the real space configuration, the magnetic ground state is an orthorhombic uniaxial stripe state. The stripe order reduces the point-group symmetry of a unit cell from C4 (tetragonal) to C2 (orthorhombic). In the nematic state, the order parameters are set to ∆x=∆y=0 and ∆x2≠∆y2. This implies that the magnetic fluctuations associated with one of the ordering vectors are stronger than the other ∆x2>∆y2 or ∆y2>∆x2. Therefore, the Z2 symmetry is broken, but the O(3) spin-rotational symmetry is not. In the real space configuration, the x- and y-directions of the magnetic fluctuations are inequivalent.
Recently, the reentrant C4 symmetry magnetic orders have been reported in hole-doped Fe-pnictide [27, 31, 32]. A double-Q order (choose both Qx and Qy) has been proposed to change the ground state from striped to tetragonal [33, 34]. Two stripe orders with the ordering vectors Qx and Qy are superposed to preserve the tetragonal symmetry. As a matter of fact, the nematic phase is characterized by an underlying electronic order that spontaneously breaks tetragonal symmetry. Since the double-Q order does not break the C4 symmetry, it is not suitable to explain the nematicity.
The magnetic fluctuations trigger a transition from the tetragonal-to-orthorhombic phase. At very high temperature, T>TS, ∆x=∆y=0, and the fluctuations of all order parameters have equal strength, i.e., ∆x2=∆y2. As the temperature lowers, TN<T<TS, the thermodynamic average of order parameters still remains ∆x=∆y=0 but ∆x2≠∆y2. The fluctuations of one of the orders ∆x are on average different from the fluctuations of the other order ∆y implying a broken Z2 symmetry and a preserved O(3) symmetry. When the temperature is below TN, the magnetic ground state is a stripe SDW state, i.e., ∆x=0 or ∆y=0.
In this chapter, we will exploit a two-orbital model to study the interplay between SC and nematicity in a two-dimensional lattice. The two-orbital model has been successfully used in many studies such as quasiparticle excitation, the density of states near an impurity [35, 36] and the magnetic structure of a vortex core [37].
2. Model
Superconductivity in the iron-pnictide superconductors originates from the FeAs layer. The Fe atoms form a square lattice, and the As atoms are alternatively above and below the Fe-Fe plane. This leads to two sublattices of irons denoted by sublattices A and B. Many tight-binding Hamiltonians have been proposed to study the electronic band structure that includes five Fe 3d orbitals [38], three Fe orbitals [39, 40], and simply two Fe bands [41, 42, 43]. Each of these models has its own advantages and range of convenience for calculations. For example, the five-orbital tight-binding model can capture all details of the DFT bands across the Fermi energy in the first Brillouin zone. However, in practice, it becomes a formidable task to solve the Hamiltonian with a large size of lattice in real space even in the mean-field level. Several studies used five-orbital models in momentum space to investigate the single-impurity problem for different iron-based compounds such as LaFeAsO1−xFx, LiFeAs, and KxFe2−ySe2. These studies confirmed that the detail of electronic bands strongly influences on the magnitude and location of the in-gap resonant states generated by the scattering of quasiparticles from single impurity [44, 45, 46].
On the other hand, the two-orbital models apparently have a numerical advantage dealing with a large size of lattice while retaining some of the orbital characters of the low-energy bands. Among the two-orbital (dxz and dyz) models, Zhang [47] proposed a phenomenological approach to take into account the two Fe atoms per unit cell and the asymmetry of the As atoms below and above of the Fe plane. Later on, Tai and co-workers [48] improved Zhang’s model by a phenomenological two-by-two-orbital model (two Fe sites with two orbitals each). The obtained low-energy electronic dispersion agrees qualitatively well with DFT in LDA calculations of the entire Brillouin zone of the 122 compounds.
The multi-orbital Hamiltonian of the iron-pnictide superconductors in a two-dimensional square lattice is described as
with σαβ the Pauli matrices. The operators ciuα† (ciuα) create (annihilate) an ectron with spin α,β=↑,↓ in the orbital u,v=1,2 on the lattice site i; tijuv is the hopping matrix element between the neighbor sites, and μ is the chemical potential. U (U′) is the intraorbital (interorbital) on-site interaction. Hund’s rule coupling is JH and the pair hopping energy is J′. The spin-rotation invariance gives U′=U−2JH and J′=JH [49]. Repulsion between electrons requires JH<U∕3.
Here, we adopt Tai’s phenomenological two-by-two-orbital model because it is able to deal with a large size of lattice in many aspects and the details of low-energy bands are similar to the results from DFT + LDA. In a two-orbital model, the hopping amplitudes are chosen as shown in Figure 1 [48] to fit the band structure from the first-principle calculations:
(color online) two-dimensional square lattice of the iron-based superconductors. There are two Fe atoms (green and gray color) in a unit cell, and each atom has two orbitals. The bright color circle represents the first orbital, and the faded color circle represents the second orbital. Solid lines indicate the hopping between the atoms in the same orbital and dashed lines indicate the hopping between the atoms in the different orbitals.
Figure 1 shows the hopping parameters between unit cells and orbitals. For the same orbital, the hopping parameters t2 and t3 are chosen differently along the mutually perpendicular directions. The C4 symmetry on the same orbital between different sublattices is broken. However, t2 and t3 are twisted for the different Fe atoms on the same sublattice which restore the C4 symmetry of the lattice structure.
In the mean-field level
H=H0+H∆+Hint,E10
the Hamiltonian is self-consistently solved accompanied with s+−-wave superconducting order. The mean-field scheme is the same as Ref. [48]:
The next nearest-neighbor intraorbital attractive interaction V is responsible for the superconducting order parameter Δijuu=Vci↑cj↓ [50, 51, 52]. According to the literatures where U is chosen to be 3.2 or less [48, 52], the magnetic configuration is a uniform SDW order. In order to make the stripe SDW order and the nematic order by changing electron doping, i.e., the chemical potential μ, we choose the parameters of interactions U=3.5, JH=0.4, and V=1.3 to induce a nematic order within a small doping range.
In momentum space, the spin configuration is determined by the order parameters ∆x and ∆y. The combination of these order parameters lacks the visualization of the magnetic structure in real space. Therefore, we choose the staggered magnetization Mi in a lattice to study the states driven by the magnetic mechanism. The magnetic configuration is described as
Mi=M1cosqy·rieiQx·ri+M2sinqx·rieiQy·ri,E14
where the wave vectors qx=2π/λ0 and qy=02π/λ correspond to a modulation along the x-axis and the y-axis with wavelength λ. M1 and M2 are the amplitude of the modulation.
In the case of the absence of both qx and qy, Mi becomes
Mi=M1eiQx·ri+M2eiQy·ri.E15
As M1=0 or M2=0 is chosen, i.e., choosing the ordering vector either Qx or Qy, the state is a stripe SDW state. The existence of qx and qy does not affect the stripe SDW state. As two values of M1 and M2 are arbitrarily chosen, the spin configuration forms a stripe SDW along the 11 direction. The existence of qx and qy has a lot of influences on the nematic state.
In the nematic state, the presence of both Q and q ordering vectors is necessary. Unlike the double-Q model, with the choice M1≠M2, the magnitudes of the modulated antiparallel spins along the x-axis and the y-axis are different due to the existence of q vectors. The magnetic configuration is attributed to two inequivalent stripes interpenetrating each other and formed a checked pattern. The checked pattern has the same period along the x- and y-directions. The period is determined by the value of q in the periodic boundary conditions. The value of q, therefore, cannot be arbitrary and must commensurate the lattice to stabilize the modulation and lower the energy of the system. As two modulated stripes have no phase difference, the checked patter shows a s-wave-like symmetry. In addition, as the modulations have a phase shift of π/2, the checked pattern shows a d-wave-like symmetry.
Figure 2 displays the Fermi surface and the band structure in the absence of SDW at the normal state, i.e., the superconductivity is set to zero. In the absence of SDW U=0, the Hamiltonian in momentum space is
(color online) (a) and (b) are, respectively, the band structure and the Fermi surface without SDW. The Fermi energy (red dashed line) corresponds to the electron filling n=2.1.
The eigenvalues are
E1,k=ε¯+−ε¯−2+ε12−εAB2−εc−μ,E25
E2,k=ε¯++ε¯−2+ε12−εAB2−εc−μ,E26
E3,k=ε¯+−ε¯−2+ε12+εAB2+εc−μ,E27
E4,k=ε¯++ε¯−2+ε12+εAB2+εc−μ,E28
where
ε¯±=εA1±εB12.E29
Figure 2(a) shows that two hole bands are around the Γ point and two electron bands are around the M point. There is no gap in the band structure where the superconductivity is able to open a gap. The nature of Fermi surface is revealed by the line at the Fermi energy crossing the band dispersion through Γ−X−M−Γ points. Figure 2(b) displays that the Fermi surface contains two hole pockets that are centered at Γ point and two electron pockets that are centered at M points. In addition, the Fermi surface also exhibits the C4 symmetry of the lattice structure.
In the stripe SDW state, the spin configuration is shown as Figure 3. The stripe SDW order enlarges the two-Fe unit cell to four-Fe unit cell as denoted by the blue dashed square in Figure 3. The antiferromagnetic order is along the X′-axis and the ferromagnetic order is along the Y′-axis. The magnetic unit cell (four-Fe unit cell) with lattice spacing 2a is oriented at a 45° angle with respect to the nonmagnetic unit cell (two-Fe unit cell). The magnetic Brillouin zone is a square oriented at a 45° angle with respect to the crystal Brillouin zone. The size of the magnetic unit cell is twice of the nonmagnetic unit cell, and the size of the magnetic Brillouin zone is half of the crystal Brillouin zone. The Hamiltonian in momentum space is
(color online) the schematic lattice structure of the Fe layer in the stripe SDW state. Blue dashed square denotes the four-Fe unit cell in the stripe SDW state.
According to the itinerant picture, the interactions between two sets of pockets give rise to a SDW order at the wave vector connecting them with Qx=π0 or Qy=0π. For example, as choosing the ordering vector Qx, the spin configuration has antiparallel spins along theX′-direction and parallel spins along the Y′-direction [35]. The antiferromagnetism causes the gapless structure along the X′-direction, and the ferromagnetism opens a gap along the Y′-direction, as shown in Figure 4(a). There are four pockets centered at the Γ point, and two pockets along the Γ−Y′ direction are inequivalent to other two pockets along the Γ−X′ direction. The C2 symmetry of the Fermi surface resulting from the SDW gap is shown in Figure 4(b).
Figure 4.
(color online) (a) and (b) are, respectively, the band structure and the Fermi surface in the stripe SDW state. The Fermi energy (red dashed line) corresponds to the electron filling n=2.04. X′ and Y′ indicate the magnetic Brillouin zone of the stripe SDW state.
In the nematic state, the antiparallel spins are along both the X′′andY′′ directions. The nematic unit cell is oriented at a 45° with respect to the nonmagnetic unit cell. The nematic Brillouin zone is also a square oriented at a 45° angle with respect to the crystal Brillouin zone. Since the antiferromagnetism is along both the X′′andY′′directions, there is no gap in the band structure. In addition, asM1<M2, the bands along the Y′′direction are lifted higher and cause the bands to be asymmetric with respect to the Γ point. The asymmetric bands result in deformed Fermi surfaces near the Γ point. As shown in Figure 5(a), the blue curve in the band structure forms an elliptic hole-pocket Fermi surface. Furthermore, the elliptic Fermi surface results from the unequal contribution of two orbitals dxz and dyz. The mechanism behind the fluctuations of dxz and dyz orbitals can be understood from an extended RPA approach where dxz, dyz, and dxy orbitals equally contribute to the SDW instability, and in particular the dxy orbital plays a strong role in the nematic instability [30]. The nematic instability breaks the degeneracy of two orbitals dxz and dyz and causes the unequal charge distributions nxzk and nyzk. The C2-symmetry of the Fermi surface results from the broken degeneracy of two orbitals dxz and dyz (blue and red curves in Figure 5(b)).
Figure 5.
(color online) (a) and (b) are, respectively, the band structure and the Fermi surface in the nematic state. The asymmetric band (blue color) is responsible for the elliptic Fermi surface around the Γ point. The blue and red solid curves represent the major contributions from the orbitals dxz and dyz, respectively. The chemical potential is chosen as the electron filling n=2.1. X′′, and Y′′ indicate the magnetic Brillouin zone of the nematic state.
Recently, Qureshi et al. [53], Wang et al. [54], Steffens et al. [55], and Luo et al. [56] pointed out that in-plane spin excitations exhibit a large gap and indicating that the spin anisotropy is caused by the contribution of itinerant electrons and the topology of Fermi surface. These experiments indicate that the elliptic spin fluctuations at low energy in iron pnictides are mostly caused by the anisotropic damping of spin waves within FeAs plane and the topology of Fermi surface. The degeneracy of orbitals will introduce the single-ion anisotropy in spin fluctuations.
3. Visualize nematicity in a lattice
To visualize the nematicity in a lattice, we self-consistently solve the Bogoliubov-de Gennes (BdG) equations for the nematic state in a two-dimensional square lattice:
In Figure 6, we show the magnetic configuration in the coexisting state of the nematic order and SC. To view the detail of the structure, the slided profile along the peaks along the x- or y-direction is made (as shown on the sides of Mi in Figure 6). There are two sinusoidally modulated magnetizations on each panel. The warm color and cold color modulations represent the spin-up modulation and the spin-down modulation, respectively. The amplitude of each modulation on the left and right panels corresponds to the value of M1 and M2. On the left panel, we have M1cosqy·ri=0.04cos2πri28a, and on the right panel, we have M2cosqx·ri=0.06sin2πri28a. Both modulations have the same period 28a. Since M1<M2, the configuration is orthorhombic and breaks the 90° rotational symmetry.
Figure 6.
(color online) the real space configurations of the magnetization Mi are plotted on a 56×56 square lattice. The left and the right panels are the sliced profile along the peaks along the y- and x-directions, respectively. Two curves are shown in both panels. The upper and lower curves represent the spin-up and spin-down configurations, respectively.
Figure 7 shows the Fourier transformation of the spatial configuration of the nematic fluctuations. Two peaks appearing at ±π0 correspond to the ordering vector Qx and two peaks exhibiting at 0±π correspond to the ordering vector Qy. We found that the intensities of peaks associated with the ordering vector Qx are greater than peaks associated with the ordering vector Qy, which is due to the unequal value of M1 and M2. The intensities of two peaks along the kxky-direction have the same magnitude indicating ∆x=∆y=0. Moreover, the nonequivalence of the intensities between the kx- and ky-directions indicates ∆y2>∆x2. Therefore, the modulated antiparallel spin configuration is the nematic state. These features are preserved even as the SC order is equal to zero. This result is in agreement with the neutron scattering experiments [3, 10].
Figure 7.
(color online) the Fourier transformation of the 56×56 spatial magnetic configuration.
We further illustrate the electronic charge density ni=ni↑+ni↓ and the s+−-wave SC order parameter Δi as shown in Figure 8(a), (b). Particularly, the nematicity of the spin order induces a modulated charge density wave (CDW) which does not occur in the stripe SDW state. The CDW consists of crisscrossed horizontal and vertical stripes. The amplitudes of the vertical stripes are larger than the horizontal stripes. Therefore, the CDW forms a checked pattern, instead of a checkerboard pattern. The stripes on both x- and y- directions have the same period 14a which is the half period of the magnetization.
Figure 8.
(color online) (a) the spatial configuration of the electronic charge density ni. (b) the spatial configuration of the s+−-wave superconducting order parameter Δi.
Moreover, although the checked pattern of the CDW is twofold symmetry, the CDW exhibits a dx2−y2-symmetry, instead of a dxy-symmetry (diagonal stripes crisscrossed pattern), form factor density wave. The space configuration of the SC order parameter Δi shows the same features as the CDW order, as shown in Figure 8(b).
4. The local density of states
The local density of states (LDOS) proportional to the differential tunneling conductance as measured by STM is expressed as
ρiE=−1NxNy∑nuuiu↑n2f′En−E+viu↓n2f′En+E,E50
where Nx×Ny=24×24 is the size of supercells.
In the striped SDW state, spins are parallel in the y-direction and antiparallel in the x-direction and cause the gap and gapless features in the band structure, respectively. The SDW gap shifts toward negative energy, and the coherence peak at the negative energy is pushed outside the SDW gap and enhanced. The coherence peak at the positive energy is moved inside the SDW gap and suppressed. This is a prominent feature caused by the magnetic SDW order that the intensities of superconducting coherence peaks are obvious asymmetry (as shown in Figure 9(a)) [57].
Figure 9.
(color online) the LDOS in the (a) stripe SDW state and (b) nematic state. The dashed (blue) line represents the LDOS without magnetization (Mi=0).
In the nematic state, spins are antiparallel in the x- and y-directions leading to a gapless feature in the band structure. The superconducting gap is the only gap that appears in the LDOS. Moreover, comparing to the state without SDW, the competition between the nematic order and the superconducting order causes the slightly suppression of the coherence peaks. The feature of the suppression results in a dip at the negative energy outside the coherence peaks (as shown in Figure 9(b)).
Furthermore, Figure 10 displays a spatial distribution of LDOS, also known as LDOS map, at E=0.14. The LDOS map shows the same features as the charge density distribution at the energy within the coherence peaks. The LDOS map exhibits a checked pattern, twofold symmetric configuration, and dx2−y2-symmetry form factor density wave. These features have not yet been reported by STM experiments.
Figure 10.
(Color online) The LDOS map at E=0.14 with Mi≠0.
It is worth to note that STM measurements by Chuang et al. [5] and Allan [58] reported that the dimension of the electronic nanostructure is around 8a and the nanostructure aligns in a unidirectional fashion. The highly twofold symmetric structure of the QPI patterns is represented by using the Fourier transformation of the STS imaging. Moreover, in cuprate, the more advanced measurement of the atomic-scale electronic structure has shown a d-wavelike symmetry form factor density wave [59, 60]. There are four peaks that appear around the center of the momentum space in the QPI patterns. Such an atomic-scale feature in cuprates has not yet been reported in iron pnictides and in the nematic state.
5. Phase diagram
To further verify the spin configuration of the nematic order, a phase diagram is presented in Figure 11. In the phase diagram, the stripe SDW order, nematic order, and s+−-wave superconducting order as a function of doping are obtained from the self-consistent calculation to solve the BdG equations.
Figure 11.
(color online) the phase diagram of the stripe SDW order (blue), nematic order (green), and superconducting order (red) as a function of doping.
In the hole-doped region, the magnetization exhibits the stripe SDW order and drops dramatically around n=1.85 and vanishes at n=1.80. In the meantime, the s+−-wave superconducting order reaches its maximal value at n=1.85 and then gradually decreases.
In the electron-doped region, the stripe SDW order (green curve) has its maximal value at n=2.00, then rapidly diminishes in a small region of doping, and finally reaches zero at n=2.09. The superconductivity (blue curve) swiftly increases in a small region from n=2.02 to n=2.04, then reaches its maximal value at n=2.10, and finally gradually decreases to almost zero around n=2.40. The nematic state (red region) is in a small region next to the stripe SDW where the nematic transition line (red dashed curve) tracks closely the stripe SDW transition line. The nematic order is favored to appear in the electron-doped regime, but not the hole-doped regime.
There are two regions where the stripe SDW coexist with the SC and the nematic order coexists with the SC. In the region where the stripe SDW coexist with the SC, the magnetic structure is an orthorhombic uniaxial stripe state. The ordering vector is either Qx or Qy implying ∆x=0 or ∆y=0. In the region where the nematic order coexists with the SC, the magnetic structure is a crisscrossed stripe state with twofold symmetry. The ordering vectors are Qx and Qy associated with two modulating vectors qx and qy implying ∆x=∆y=0 and ∆x2−∆y2≠0 [61].
It is worth to note that the phase diagram of the electron-doped region is consistent with Figure 1.3 of Kuo’s thesis on BaFe1−xCoxAs2 [62]. Both figures show the same behavior of the nematic phase. Near the optimally doped region under the superconducting dome, it is mentioned that the long-range nematic order coexists with the superconductivity. However, such results still have not been reported from experiments. In addition, the magnetoresistivity of Ba0.5K0.5Fe2As2 reported a nematic superconducting state recently and suggested that the hole-doped superconductor is the mixture of s-wave and d-wave superconducting orders [63]. These results provide a different path to further researches to understand the mechanism of the nematic state in the superconductivity.
6. Conclusions
The two-orbital Hamiltonian used in the iron-based superconductors has always been questioned for its validity. Many studies have approved that a lot of phenomena are attributed to dxz and dyz orbitals. In particular, dxz and dyz orbitals are responsible for the SDW instability.
The stripe SDW order opens a gap in the band structure and deforms the Fermi surface. However, the band structure of the nematic order is gapless, and the Fermi surface is deformed to an ellipse. The mechanism can be understood from the instability of SDW. The nematic order has visualized as a checked pattern formed by a crisscrossed modulated horizontal and vertical stripes. The inequivalent strengths of the horizontal and vertical stripes break the degeneracy of two orbitals dxz and dyz and cause an elliptic Fermi surface. The Fourier transformation of the orthorhombic structure of the magnetization shows two uneven pairs of peaks at (±π,0) and (0,±π). Moreover, the LDOS map shows a dx2-y2-symmetry form factor density wave.
Finally, the nematic order is favored to exist in the electron-doped regime, but not the hole-doped regime.
Acknowledgments
HYC was supported by MOST of Taiwan under Grant MOST 107-2112-M-003-002 and National Center for Theoretical Science of Taiwan.
\n',keywords:"magnetic fluctuation, stripe SDW, nematic order, two-orbital, elliptic Fermi surface, LDOS maps",chapterPDFUrl:"https://cdn.intechopen.com/pdfs/65626.pdf",chapterXML:"https://mts.intechopen.com/source/xml/65626.xml",downloadPdfUrl:"/chapter/pdf-download/65626",previewPdfUrl:"/chapter/pdf-preview/65626",totalDownloads:203,totalViews:0,totalCrossrefCites:0,dateSubmitted:"September 12th 2018",dateReviewed:"January 15th 2019",datePrePublished:"January 15th 2020",datePublished:null,dateFinished:null,readingETA:"0",abstract:"The nature of the nematicity in iron pnictides is studied with a proposed magnetic fluctuation. The spin-driven order in the iron-based superconductor has been realized in two categories: stripe SDW state and nematic state. The stripe SDW order opens a gap in the band structure and causes a deformed Fermi surface. The nematic order does not make any gap in the band structure and still deforms the Fermi surface. The electronic mechanism of nematicity is discussed in an effective model by solving the self-consistent Bogoliubov-de Gennes equations. The nematic order can be visualized as crisscross horizontal and vertical stripes. Both stripes have the same period with different magnitudes. The appearance of the orthorhombic magnetic fluctuations generates two uneven pairs of peaks at ±π0 and 0±π in its Fourier transformation. In addition, the nematic order breaks the degeneracy of dxz and dyz orbitals and causes the elliptic Fermi surface near the Γ point. The spatial image of the local density of states reveals a dx2-y2-symmetry form factor density wave.",reviewType:"peer-reviewed",bibtexUrl:"/chapter/bibtex/65626",risUrl:"/chapter/ris/65626",signatures:"Hong-Yi Chen",book:{id:"8823",title:"On the Properties of Novel Superconductors",subtitle:null,fullTitle:"On the Properties of Novel Superconductors",slug:"on-the-properties-of-novel-superconductors",publishedDate:"July 29th 2020",bookSignature:"Heshmatollah Yavari",coverURL:"https://cdn.intechopen.com/books/images_new/8823.jpg",licenceType:"CC BY 3.0",editedByType:"Edited by",editors:[{id:"24773",title:"Dr.",name:"Heshmatollah",middleName:null,surname:"Yavari",slug:"heshmatollah-yavari",fullName:"Heshmatollah Yavari"}],productType:{id:"1",title:"Edited Volume",chapterContentType:"chapter",authoredCaption:"Edited by"}},authors:null,sections:[{id:"sec_1",title:"1. Introduction",level:"1"},{id:"sec_2",title:"2. Model",level:"1"},{id:"sec_3",title:"3. Visualize nematicity in a lattice",level:"1"},{id:"sec_4",title:"4. The local density of states",level:"1"},{id:"sec_5",title:"5. Phase diagram",level:"1"},{id:"sec_6",title:"6. Conclusions",level:"1"},{id:"sec_7",title:"Acknowledgments",level:"1"}],chapterReferences:[{id:"B1",body:'Christianson AD, Goremychkin EA, Osborn R, Rosenkranz S, Lumsden MD, Malliakas CD, et al. Unconventional superconductivity in Ba0.6K0.4Fe2As2 from inelastic neutron scattering. Nature. 2008;456:930'},{id:"B2",body:'Séamus Davis JC, Lee D-H. Concepts relating magnetic interactions, intertwined electronic orders, and strongly correlated superconductivity. PNAS. 2013;110:17623'},{id:"B3",body:'Zhao J, Adroja DT, Yao D-X, Bewley R, Li S, Wang XF, et al. Spin waves and magnetic exchange interactions in CaFe2As2. Nature Physics. 2009;5:555'},{id:"B4",body:'Yi M, Donghui L, Chu J-H, Analytis JG, Sorini AP, Kemper AF, et al. 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Nature Physics. 2013;9:220'},{id:"B59",body:'Fujita K, Hamidian MH, Edkins SD, Kim CK, Kohsaka Y, Azuma M, et al. Direct phase-sensitive identification of a d-form factor density wave in underdoped cuprates. PNAS. 2014;111:E3026'},{id:"B60",body:'Hamidian MH, Edkins SD, Kim CK, Davis JC, Mackenzie AP, Eisaki H, et al. Atomic-scale electronic structure of the cuprate d-symmetry form factor density wave state. Nature Physics. 2016;12:150'},{id:"B61",body:'Chou C-P, Chen H-Y, Ting CS. The nematicity induced d -symmetry charge density wave in electron-doped iron-pnictide superconductors. Physica C. 2018;546:61'},{id:"B62",body:'Kuo H-H. Electronic Nematicity in Iron-Based Superconductors [Thesis]. Stanford University; 2014'},{id:"B63",body:'Li J, Pereira PJ, Yuan J, Lv Y-Y, Jiang M-P, Lu D, et al. Nematic superconducting state in iron pnictide superconductors. Nature Communications. 2017;8:1880'}],footnotes:[],contributors:[{corresp:"yes",contributorFullName:"Hong-Yi Chen",address:"hongyi@ntnu.edu.tw",affiliation:'
Department of Physics, National Taiwan Normal University, Taipei, Taiwan
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In case of substance loss, a nerve guide should be used to bridge the proximal with the distal stump of the severed nerve. The effectiveness of hollow nerve guides is limited by the delay of axonal growth due to the absence of a regeneration substrate inside the conduit. To fasten up nerve regeneration, nerve guides should thus be enriched by a luminal filler. In this study, we investigated, in a 12-mm rat sciatic nerve defect experimental model, the effectiveness of chitosan-based conduits of different acetylation filled either with a hyaluronic acid gel (NVR gel) or with a magnetic fibrin hydrogel, in comparison with traditional autografts. Results showed that all types of artificial nerve conduits led to functional recovery not significantly different from autografts. 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Open Access publishing helps remove barriers and allows everyone to access valuable information, but article and book processing charges also exclude talented authors and editors who can’t afford to pay. The goal of our Women in Science program is to charge zero APCs, so none of our authors or editors have to pay for publication.
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