Common laser-active rare earth ions and host media and important emission wavelengths.
Particles of sizes between 1 and 100 nm show fascinating properties with unusual characteristics that lead to the formation of unique properties in nanosystems, which are not observed in ordinary materials. These are considered hereby as nanoparticles (NPs). Additionally, metallic NPs with sizes smaller than the wavelength of light show strong dipolar excitations in the form of localized surface plasmon resonances (LSPR). LSPRs are non-propagating excitations of the conduction electrons of metallic NPs coupled to the electromagnetic field . This effect has been the subject of extensive research, both fundamental and with a view to applications [2,3]. The resonance frequency of the oscillation, i.e., the surface plasmon (SP) energy, it is essentially determined by the dielectric properties of the metal and the surrounding medium, and by the particle size and shape. The collective charge oscillation causes a large resonant enhancement of the local field inside aand near the NP. This field enhancement is used in surface-enhanced Raman scattering (SERS)  and is currently discussed for potential applications in nonlinear optical devices , in optical tweezers , and generally for the manipulation of the local photonic density of states.
Rare-earth (RE) elements are a group of chemical elements known as Lanthanides that occur together in the periodic table. These elements are used in common consumer goods such as: computer memory, DVD’s, rechargeable batteries, cell phones, car catalytic converters, magnets, fluorescent lighting and much more. Furthermore, play an essential role in modern national defense, e.g.: lanthanum in night-vision goggles, neodymium in laser range-finders, guidance systems, communications; europium in fluorescents and phosphors in lamps and monitors; erbium amplifiers in fiber-optics data transmission; samarium in permanent magnets stable at high temperatures and, others technological applications. We center our attention in the RE ions and their optical properties that are widely employed in photonic. Devices of general interest span RE ions concentrations of tens to several thousand parts per million (ppm), resulting in devices of one to tens of meters long such as channel waveguides and optical fiber, respectively. In optical devices, the RE should ideally be confined as a delta function in the center of the core for maximum gain per unit pump power. Thereby, there is a necessary tradeoff between the confinement and the RE ions concentration, such that the more confined structures require a higher rare-earth ions concentration. An important feature that distinguishes them from other optically active ions: they emit and absorb over narrow wavelength ranges, the wavelengths of the emission and absorption transitions depend the host material, the intensities of these transitions are weak, the lifetimes of metastable states are long, and the quantum efficiencies tend to be high, except in aqueous solutions. These properties lead to excellent performance of RE ions in many optical applications. Devices that provide gain (e.g. lasers and amplifiers), must have low scattering losses, and one is restricted to using single-crystal or glass hosts. Whereas in many applications crystalline materials are preferred for reasons that include higher peak cross sections or better thermal conductivities, the versatility of glasses and the broader emission and absorption spectra they provide have led to the use of RE doped glasses in many applications, eventually running into the clustering limit for the particular host glass composition .
Most of existing and potential future applications of NPs suffer from damping caused by metal absorption. Sudarkin and Demkovich  suggested increasing the propagation length of the surface plasmon polariton A SPP is an electromagnetic wave propagating along the interface between two media possessing permittivities with opposite signs, such as the metal–dielectric interface.
A SPP is an electromagnetic wave propagating along the interface between two media possessing permittivities with opposite signs, such as the metal–dielectric interface.
In the present chapter, we explore the physics of localized surface plasmons by first considering the interaction of metal NPs with an electromagnetic wave in order to arrive at the resonance condition (LSPR). After, we show studies of plasmon resonances in particles with different shapes and sizes, and the effects of interactions between particles in the ensemble. Then we will focus on the RE ions, discussing the optical properties of the trivalent ions through the principles of quantum mechanics (in terms of oscillator strengths) with special interest in the interactions between the 4f electrons themselves. Since all the other electronic shells are spherically symmetric. Finally we present diverse experimental results of the interaction of RE ions interaction with NPs, resulting in an enhancement of the intensity emission of the RE ions due to long-range electromagnetic interaction between LSPR and the RE ions.
In this context, it is worth mentioning that the main purpose of this chapter is to show some of concrete concept of
2. Localized surface plasmon resonance and metallic nanoparticles
First, we know that a surface plasmon resonance (SPR) can be described as the resonance collective oscillation of valence electrons in a solid stimulated by beam of light incident (electromagnetic field – see Figure 1). The resonance condition is established when the frequency of light matches the natural frequency of valence electrons oscillating against from this restoring force. SPR in nanometer-sized structures is called LSPR. For gold and silver NPs, the resonance falls into the visible region of the electromagnetic spectrum. A striking consequence of this is the bright colors exhibited by particles both in transmitted and reflected light, due to resonantly enhanced absorption and scattering. This effect has found applications for many hundreds of years, for example in the staining of glass for windows or ornamental cups Localized surface plasmons have been observed since the Romans who used gold and silver nanoparticles to create colored glass objects such as the Lycurgus Cup (4th Century A.D.). A gold sol in the British museum, created by Michael Faraday in 1857, is still exhibiting its red color due to the plasmon resonance at ,530 nm [L. M. Liz-Marzan, Mater. Today 7, 26 (2004).].
Localized surface plasmons have been observed since the Romans who used gold and silver nanoparticles to create colored glass objects such as the Lycurgus Cup (4th Century A.D.). A gold sol in the British museum, created by Michael Faraday in 1857, is still exhibiting its red color due to the plasmon resonance at ,530 nm [L. M. Liz-Marzan, Mater. Today 7, 26 (2004).].
2.1. Noble metal nanoparticles in an electric field
For spherical NPs smaller than compared to local variations of the involved electromagnetic fields (
Here is the (complex) polarizability of the NP in the electrostatic approximation. Under the condition thatis a minimum, the polarizability shows a resonant enhancement. Thus, we can also write the Frohlich conditionthat is the associated mode the dipole surface plasmon of the NP (in an oscillating field). Nevertheless, the distribution of the electric field inside and outside the sphere can be written as:
Here, is the dipole moment. Therefore, a resonance in implies a resonant improvement of both the internal and dipolar fields, resulting in prominent applications of NPs in optical devices. Now consider a plane wave incident with, this induce on NP an oscillating dipole moment, i.e., we have a scattering of the plane wave by the NP. In this sense, the electromagnetic fields associated with an electric dipole in the near, intermediate and radiation zones are :
With and n is the unit vector in the direction of the point P of interest. For
From the viewpoint of optics, it is much interesting to note that another consequence of the enhanced polarization in which a NP scatters and absorbs light . For a sphere of volume
2.2. Mie theory
For particles with larger dimensions, where the quasi-static approximation is not justified due to significant phase-changes of the driving field over the particle volume, a rigorous electrodynamics approach is required. This way, Gustav Mie solved Maxwell’s equations for the case of an incoming plane interacting with a spherical particle . In essence, the electromagnetic fields are expanded in multipole contributions and the expansion coefficients are found by applying the correct boundary conditions for electromagnetic fields at the interface between the metallic NP and its surrounding.
The extinction cross section of a spherical NP is given by the following expression:
Here the parameters
The size parameter
We will focus our attention in silver and gold, since the localized plasmon resonance condition mentioned above is satisfied at visible light frequencies. Additional advantages of these metal NPs include simple preparation methods for a wide range of sizes and shapes and easy surface conjugation to a variety of ligands.
We now evaluate the extinction cross section using the Mie theory from equation (9), Figure 2, we take dielectric constants for silver and gold from Palik , and the medium dielectric constant is assumed to be 1.0 (i.e., a particle in a vacuum) and 2.0 for NPs with sizes different.
We can see from Figure 2 the dependence of resonance frequency with size of NPs (silver and gold) and the refraction index (surrounding medium). K. Lance Kelly et al. (2003), show that for spherical NPs clear differences between the quasistatic and the Mie theory results. However, the important features are retained, e.g. the frequency resonance. Although Mie theory is not a very expensive calculation, the quasistatic expressions are convenient to use when only qualitative information is needed .
Now, Figure 3 shows clearly the dependence of resonance frequency embedded in a glass (with refraction index of: 1.99 for 400 nm, 1.88 for 630 nm, 1.75 for 900 nm and 1.70 for 1000 nm) and in a bulk with refraction index 2, in both cases with 20 nm size and a size distribution of 20 % STD, this simulation was extracted from program MiePlot v4.2.11 of Philip Laven. Also, it is possible to observe an increment of bandwidth and the intensity of peak for NPs embedded in the glass when compared with the material bulk. Therefore, LSPR results in enhanced local electromagnetic fields near the surface of the NP (Novotny & Hecht, 2006) , see Figure 1.
Hideki Nabika and Shigehito Deki , show an experimental evidence of this dependence above mentioned for silver NPs of different sizes were synthesized by reducing AgNO3 with N,N-dimethylformamide (DMF), Poly(vinylpyrrolidone) (PVP) aqueous solution (10 mL, 10 wt %) was added to DMF (80 mL), followed by an addition of AgNO3 aqueous solution (10 mL). They obtained three sets of spherical silver NPs with a particle diameter varying from 9.7 to 27.1 nm and rod-shaped silver NPs with an aspect ratio of 1.79, its results are show Figure 4.
Thereby, the LSPR properties are sensitive to its environment in the order of its shape and size , the dielectric function of the glass host containing the NPs, changes the LSPR bandwidth and resonance frequency, see Figure 2-4.
We can be written as the sum of the bound and quasi-free (conduction) electron contributions :, is the damping the resonance, ω the excitation frequency,
On the other hand, in the Gans theory, the LSPR is only a function of the aspect ratio and refractive index. Thus, in certain conditions, a linear relationship between them can be resulted . Nevertheless, numerical results suggest that, even when the aspect ratio is fixed and the retardation effect is weak, the position of longitudinal resonance can still depend strongly with the aspect ratio [29, 30]. Using the model of Cheng - ping Huang et al , we can write:
Where = l/2r is the aspect ratio of the NPs (with the inner radius r and in a cylindrical region with the length l), and is the skin depth. Cheng - ping Huang considered the problem as using an LC circuit model without solving the Laplace or Maxwell equations, and show that its results overcomes the deficiency of Gans theory and provides a new insight into the phenomenon. This way, we can observe resonance wavelength change with the aspect ratio of NP, Figure 5. This means a breakdown of the linear behavior presenting oscillations electrons originating from the amorphous geometry of the NPs associated with the inertia of electrons, see inset Figure 2 as well.
Figure 6 illustrates this further, via experiments of X. Lu et al.  and Mock et al. . Panel (a) the nanobar Ag NPs and the corresponding dark-field light scattering spectra, in broad agreement with the simulated results shown in . Panel (b) shows the dipolar plasmon lineshapes of colloidal silver NPs of different shapes .
2.3. Coupling between metallic nanoparticles
We can say that the localized plasmon resonance frequency of a single metallic NP can be shifted through of alterations in shape, size and surrounding medium from the Frohlich condition, section 2.1. Nevertheless, in a NP ensembles we can obtain additional shifts due to electromagnetic interactions between the localized modes, see Figure 3 and 4 (c). These interactions are basically of a dipolar nature (when d<<). So, the NP ensemble can be treated as an ensemble of interacting dipoles (in a first approximation). Those NPs can be embedded into a host matrix ordered or random, in one-, two- or three-dimensional arrays with interparticle spacing D. Electromagnetic coupling of those arrays shows interesting localization effects for closely spaced particles such as, enhancement process due to field localization in NP junctions. Assuming a dipolar approximation the NPs can be treated as point dipoles. In this sense, two regimes have to be distinguished (i) For D<<, near-field interactions with a distance dependence of D
Therefore, the maximum field enhancement is determined by the shortest distance between two equipotential particles.
Figure 7 shows the near field coupling between NPs. Here, the restoring force acting on the oscillating electrons of each NP in the chain is either increased or decreased by the charge distribution of neighboring particles. Depending on the polarization direction of the exciting light, this leads to a blue-shift of the plasmon resonance for the excitation of transverse modes, Figure 7 (a) , and a red-shift for longitudinal modes, Figure 7 (b).
Today, there are several theoretical methodologies available to describe the interaction among the metallic NPs with electromagnetic radiation [33,34,35,36,37,38,39,40].
Rare earths ions in solids are either divalent or trivalent. Their electronic configuration is 4fN5s25p6 or 4fN-15s25p6, respectively. By far the most common valence state of the RE ions in solids is the trivalent one. Those ions have a long history in optical and magnetic applications. We have special interest in the devices luminescent using crystal, powders, and glasses. On the other hand, divalent RE ions have also been used in laser devices, but only in relatively exotic ones for cryogenic operation [41,42]. The most frequently used laser-active RE ions and host media together with typical emission wavelength ranges are shown in the table 1:
|Neodymium (Nd3+)||YAG, YVO4, YLF, silica||1.03–1.1, 0.9–0.95, 1.32–1.35|
|Ytterbium (Yb3+)||YAG, tungstates, silica||1.0–1.1|
|Erbium (Er3+)||YAG, silica, tellurite, chacogenetos glasses||1.5–1.6, 2.7, 0.55|
|Thulium (Tm3+)||YAG, silica, fluoride glasses||1.7–2.1, 1.45–1.53, 0.48, 0.8|
|Holmium (Ho3+)||YAG, YLF, silica||2.1, 2.8–2.9|
|Praseodymium (Pr3+)||silica, fluoride glasses||1.3, 0.635, 0.6, 0.52, 0.49|
|Cerium (Ce3+)||YLF, LiCAF, LiLuF, LiSAF, and similar fluorides||0.28–0.33|
The 4f electrons are not the outermost ones. They are shielded from external fields by two electronic shells with larger radial extension (5s25p6), which explains the atomic nature of their spectra absorption/emission, Figure 8. Thus the 4f electrons are only weakly perturbed by the charges of the surrounding atoms. Important characteristics that distinguish them from other optically active ions are: (i) the wavelengths of the emission and absorption transitions are relatively insensitive to host material, (ii) the intensities of these transitions are weak, (iii) the lifetimes of metastable states are long and, (iv) the quantum efficiencies tend to be high. This is why the RE ions are such a useful probe in a solid; the crystal environment constitutes only a small perturbation on the atomic energy levels, and many of the solid state, and hence spectroscopic, properties can be understood from a consideration of the free ions. In turn, the wavefunctions of the free ions constitute a good zero order approximation for a description of solid-state properties, Figure 8.
The solutions to this problem can then befactored into a product of a radial and angular function. Whereas the radial function depends on the details of the potential the spherical symmetry ensures that the angular component is identicalwith that of a hydrogen atom and can be expressed as spherical harmonics. Except for Ce3+ and Yb3+, which have only one electron, the solutions of the central-field problem are products of one-electron states that are antisymmetric under the interchange of a pair of electrons, as required by the Pauli exclusion principle.
In describing the state of a multielectron atom, the orbital angular momenta and the spin angular momenta are added separately. The sum of the orbital angular momenta is designated by the letter L, and the total spin is characterized by S. The total angular momentum J of the atom may then be obtained by vector addition of L and S. The collection of energy states with common values of J, L, and S is called a term. Here, the Russell-Saunders notation for the energy levels (terms) is used,
Where N=1…14 is the number of the 4f electrons, Z
Where is the potential in which the electron i is moving. The first two terms of the Hamiltonian (equation (13)) are spherically symmetric and therefore do not remove any of the degeneracies within the configuration of the 4f electrons, therefore we can neglect. The next two terms, which represent the mutual Coulomb interaction of the 4f electrons (H
Figure 8 shows the radial distribution functions 4f, 5s, 5p, and 6s electrons for Gd+ as obtained from Harteww-Fock calculation by Freeman and Watson . We can see that the 4f electrons are inner electrons with relatively small <r
3.1. Trivalent ions in a static crystal field
The 4f shell of the RE ions are an unfilled shell and therefore have a spherical charge distribution. If the ion is introduced into a crystal, the ion experiences an inhomogeneous electrostatic field, the so-called crystal field, which is produced by the charge distribution into the crystal. This crystal field distorts the closed shells of the RE ion. Producing an effect on the energy level 4f, i.e., removes to a certain degree the degeneracy of the free ion 4f levels, thus producing a major modification of the energy levels (but this depends on the crystal symmetry). In the luminescence spectrum are observed additional transitions, which originate from the excited crystal field levels of the ground term is evident, and the spectra look more complicated. On the other hand, these spectrums can be used to determine the crystal field energies of the ground term.
We shall now try to understand the behavior of these additional transitions. To do so we draw on our treatment of the Coulomb interaction of the 4f electrons. The crystal field interaction comes by the interaction of the 4f electrons with all the charges of the crystal with all charges of the crystal, except for trivial factors, it is therefore given by one over the radius vector between the 4f electrons and the crystal charges. This function is given, apart from radial factors, of two spherical harmonics, one containing the coordinates of the 4f electrons, the other containing coordinates of the crystal charge. The latter has to be integrated over the whole crystal, whereupon it gives the strength of the crystal potential at the site of the RE ion. Finally, this shows the existence of the splitting telling us that the development of the crystal potential into spherical harmonics contains a second order term.
3.1.1. Crystal field splitting
Crystal field splitting has two aspects: (i) symmetry, namely, the number of the levels into which an ion is free the J term are split in a crystal field of a given symmetry; (ii) the actual size of the crystal field splitting.
This way, the point charge model can be used for illustrative purposes but not for a quantitative description of the crystal field interaction. A realistic description of this interaction must take into account that the crystal field is built up of the spatially extended charge clouds of the individual ions. Thus, these charge clouds can penetrate each other and thereby interact. Hence, we can considered the following elements:
The ions are considered static in the crystal, i.e., we can neglected the lattice vibrations and their effect on the energy levels.
We regard the 4f electrons of one RE ion, as representative of those of all the RE ions in the crystal and, thus the interaction of 4f electrons of adjacent ions is neglected.
The crystal consists of the extended charge distributions. This produces an overlap of the charge distributions of the neighboring ions and the 4f electrons. Aditionally, a charge transfer between 4f electrons and the electrons of the ligands can take place. Both contribute to the crystal field interaction.
The 4f electrons of one ion are considered to be independent of each other, that is correlation effects play no significant role.
Therewith, we can calculate the crystal potential at the site of the 4f electrons and the potential energy of the 4f electrons in this potential. If the crystal has charge density and the 4f electrons have radius r
Where the crystal field parameter B
In early treatments of the crystal fiel interaction it was assumed that in RE compounds the point charge contribution would be the dominant part of the crystal field interaction. Then, in equation (16) the integral over the lattice can be replaced by a sum over all lattice points and can be replaced by. The latter replacement can be performed as long as the charge distribution of the crystal does not enter that of the 4f electrons (as long as r
Figure 9 further illustrates the effect of spin–orbit and crystal field interactions on the energy levels of the Er3+ ion. This figure were extracted from A.J. Kenyon . A further splitting of the energy levels comes about when the ion is placed in a silica host. The 4fN configuration is composed for a number of states where the quantum numbers (L, S, J, and another arbitrary one) define the terms of the configuration, all of which are degenerate in the central-field approximation, as illustrated in Figure 9. Next in the hierarchy is spin–orbit, the strongest of the magnetic interactions. Spin–orbit lifts the degeneracy in total angular momentum and splits the LS terms into J levels, Figure 9.
We can see that the environment provided by silica hosts destroys the spherically symmetric environment that Er3+ ions enjoy in the vapor phase. Thus the degeneracy of the 4f atomic states will be lifted to some degree. This splitting is also referred to as stark splitting, and the resulting states are called Stark components (of the parent manifold). The even-k terms in the expansion split the free ion J multiplets into Stark components generally separated by 10–100 cm-1 (see Figure 9). The ion–lattice interaction can mix multiplets with different J values (J mixing), although it usually remains a good quantum number. The odd-k terms admix higher lying states of opposite parity [e.g., 4fN15d1] into the 4fN configuration. This admixture does not affect the positions of the energy levels, but it has a very important effect on the strengths of the optical transitions between levels.
3.2. Optical properties
In recent years most of the interest in luminescent RE ions has concentrated on the trivalent erbium (Er3+), and in particular its emission band around 1550 nm. This emission is within the telecommunication windows, and fortuitously coincides with the 1550 nm intra-4f 4I13/2→4I15/2 transition of the Er3+ ion.
For this reason exists today a great interest in utilizing erbium-doped materials for gain elements and sources in telecommunications systems [48,49,50]. The development of the erbium-doped fiber amplifier (EDFA) in the late 1980s [51,52] exploited the 4I13/2→4I15/2 transition and allowed the transmission and amplification of signals in the 1530–1560 nm region without the necessity for expensive optical to electrical conversion . Hence, it is originated a driving force for research in RE doped fibers and integrated optics waveguides has been their use for amplifying weak signals in optical communications systems at 1300 and 1600 nm. This may be achieved by simply splicing a section of RE-doped fiber into the transmission one and injecting pump light through a fiber coupler. The signal generated within the RE emission band stimulates emission of radiation at the same frequency, amplifying the optical communication signal with high gain, high efficiency and low noise, which is highly advantageous for optical communications . There are five main RE candidates for use as dopants in fiber or waveguide amplifiers for optical communications systems: Er3+, Tm3+, Nd3+, Pr3+ and Dy3+. The Er3+ and Tm3+ ions are the choice for the 1400–1600 nm window centered at 1550 nm, based on the 4I13/24I15/2 transition of Er3+ ion and the 3H43F4 transition of Tm3+ ion. The 4F3/24I13/2 emission of Nd3+ ion, the 1G43H5 transition of Pr3+ ion and the 6F11/2(6H9/2)6H15/2 transition of Dy3+ ion are all potentially useful for the 1300 nm telecommunication window.
Further, the 3+ ions all exhibit intense narrow-band intra-4f luminescence in a wide variety of hosts, and the shielding provided by the 5s2 and 5p6 electrons (see Figure 8), which means that rare-earth radiative transitions in solid hosts resemble those of the free ions and electron–phonon coupling is weak. Although some of the divalent species also exhibit luminescence (e.g., samarium and europium), it is the trivalent ions that are of most interest.
As mentioned previously, the intra-4f transitions are parity forbidden and are made partially allowed by crystal field interactions mixing opposite parity wavefunctions, resulting in luminescence lifetimes long (often in the millisecond range), and linewidths narrow. The selection of an appropriate ion with intense and narrow-band emission can be obtained across much of the visible region and into the near-infrared. Figure 10 shows energy level diagrams for the isolated 3+ ions of each of the 13 lanthanides with partially filled 4f orbitals.
Almost all the RE ions their emission is due to optical transitions within the f-manifold (e.g. Tb3+ (4f8), Gd3+ (4f7) and Eu3+ (4f7). The 4f-electrons are well shielded from the chemical environment and therefore have almost retained their atomic character. Nevertheless, for a number of RE ions, also broad emission bands are known. Prominent examples are Eu2+ and Ce3+. Here, the emission is from to 5d-4f optical transitions. As electrons participate in the chemical bonding, the d-f emission spectra consist of broad bands. These transition types are allowed and are consequently very fast (a few µs or less).
Some line emission is not a specific property of RE ions and in addition to that, in the case of RE ions, broad emission spectra can be obtained as well, depending on the optical transitions involved. In this respect, RE ions are not unique. The unique properties of the RE ions originate from the fact that the spectral position of the emission lines is almost independent of the host lattice, in contrast to line emission generate by the emission of metal ions.
3.2.1. Radiative transitions: Intensities of optical transitions
The terms shown in equation (13) are time-dependent; thereby, they do not lead to stationary states of the system. This way, they are treated using time-dependent perturbation theory resulting in transitions between the states established by the static interactions. In luminescent devices the most important term is V
The experimental data on spectra of RE ions show that the radiation is mostly electric dipole (ED) nature, though some cases of the magnetic dipole radiation are also observed. Since the optical transitions take place between levels of a particular 4fN configuration, the electric dipole radiation is forbidden in first order, because the electric dipole operator has uneven parity and the transition matrix element must have even parity (Laporte selection rules). Van Vleck  pointed out the dipole electric radiation can only occur because the 4fN states have admixtures of 4fN-1nl configuration (nl will be mostly 5d), thus the 4fN-1nl has to be chosen such that it has opposite parity from 4fN. The admixture is produced via interactios that have odd parity and this depend of the host matrix of the RE ions. However, we can have four dominant sources of optical radiation in RE ions spectra:
Forced electric dipole induced by odd terms of the crystal field.
Forced electric dipole radiation induiced by lattices radiation.
Allowed magnetic dipole transition.
Allowed electric quadrupole radiation.
In free atoms, magnetic dipole is about six orders of magnitude weaker than the electric dipole radiation. This latter occurs only as a consequence of a perturbation, both kinds of radiation shows up in the RE spectra with about intensity. Then, quadrupole radiation are less probable still in comparison with the magnetic dipole.
There are different types of transitions between levels (called electric dipole, electric quadrupole, and magnetic dipole) and therefore the transitions are divided into allowed ones (with a high probability) and so-called forbidden transitions (for transitions where the electric dipole transition is quantum mechanically forbidden).
For the first order allowed magnetic dipole radiation the free atom selection rules are still quite valid:. In the electric dipole case we have:, , ,. However, since ED transitions is induced by the crystal field, the free atom selection rules break down almost completely, i.e., the selection rules with regard to the L, S and J quantum numbers are now essential governed by the crystal field interaction yielding (approximately). For the electric quadrupole case the rules selection is:.
We now outline the Judd-Ofelt theory for the determination of the intensities in RE crystal spectra [56,57]. It is in essence a quantification of the ideas formulated by van Vleck  under optical radiation sources. Intensities are often expressed in terms of oscillator strengths, where the total oscillator strength for a transition from an energy level a to an energy level b is given:
Here h is the Planck constant, the frequency of the transition ab, n the refraction index of host. S
Theparameters have so far been assumed to arise solely from crystal field; however, they also contain contributions from admixtures by the lattice vibrations. The asterisk means that forthe radial integral is to be taken between states 4f and nl instead of 4f and 4f.
Also, it is interesting to determine the coefficient for spontaneous light from state ato state b. Those are defined as:
Here c velocity of light in vacuum. The Judd-Ofelt formalism has been applied to the analysis of a number of systems. In most of these analyses the crystal field splitting of the terms is neglected; therefore, the total absorption intensities between the ground term and the excited terms are analyzed with only three empirical parameters.
If b is an excited state that decays only by the emission of photons, its observed that relaxation rate is the sum of the probabilities for transitions to all possible final states. The total rate is the reciprocal of the excited-state lifetime
The branching ratio β
The branching ratio, which has an important influence on the performance of a device based on a particular transition, appears often in the discussion of specific ions. It has a significant effect on the threshold of a laser and the efficiency of an amplifier.
4. Metallic nanoparticle embedded in a gain media: LSPR interaction radiative transitions
The RE-doped laser crystals and glasses are among the most popular solid-state gain media. In order of maintaining the efficiency of these materials in which the RE dopant is uniformily dispersed, as in multi-component glasses. In this sense, glasses have good optical, mechanical, and thermal properties to withstand the severe operating conditions of optical amplifier. Desirable properties include hardness, chemical inertness, absence of internal strain and refractive index variations, resistance to radiation-induced color centers, and ease of fabrication. Furthermore, the matrix host composition affects the solubility of the RE dopant, this affect the lifetime, absorption, emission, and excited state absorption cross sections of the dopant transitions . This competing absorption phenomenon can seriously diminish the efficiency of an optical device. For example, a decrease in the excited-state absorption for Er3+-doped fibers going from a germane-silicate host to an alumina-silicate host has been verified , demonstrating the importance of host selection for a given RE ion or laser transition. Host glasses compatible with this relatively high concentration of RE without clustering require the open, chain-like structure of phosphate glasses or the addition of modifier ions (Ca, Na, K, Li, or other) to open the silicate structure and increase solubility . The limitation owing to clustering in a predominantly silica host without modifier ions has been well documented . The maximum erbium concentration in silica for optimum amplifier performance has been suggested to be lesser to 100 ppm . However a 14.4-dB gain, 900-ppm erbium-doped silica fiber amplifier has been reported, indicating that higher concentrations can produce useful devices . Nevertheless, the interactions between host and RE ions, it is necessary to consider background losses from impurity absorption and scattering mechanisms that decrease the efficiency of the optical device. For example, depending on the phonon energies of the host matrix, some of the level lifetimes can be strongly quenched by multi-phonon transitions. Such effects are minimized in low-phonon-energy host media such as fluoride fibers. The effect of internal loss is most dramatic in distributed amplifiers, where pump light must travel long distances in the process of distributing gain.
Additionally, into the glass matrix can happen diverse kinds of interactions, in particular dipole–dipole interactions between the RE ions similar or of different species, allow energy transfer between those. This is exploited e.g. in Er3+–Yb3+-codoped fibers, where the pump radiation is dominantly absorbed by Yb3+ ions and mostly transferred to Er3+ ions .
In this way, RE-doped glasses shown are excellent materials that provide gain media. This makes them ideal candidates for embedding metallic NPs, resulting in new materials for the fabrication of devices optical with large enhancements even when the gain is saturated due light localization effects. It has been shown theoretically and experimentally that homogeneous aggregates of structures supporting LSPR can lead to extremely large enhancement of local field amplitudes exceeding those of single structures [60,61]. Besides, inorganic glasses are the host matrix for metallic NPs formation. The wide temperature range of glass viscosity growth provides the possibility to control over the NPs size within the wide range by means of modifying the temperature and duration of thermal processing. In fact, only such kind of matrix makes it possible to control and investigate all the stages of NPs formation, including the starting stage [14,62].
The LSPR in metallic NPs is predicted to exhibit a singularity when the surrounding dielectric medium has a critical value of optical gain . This singularity is obtained from the equation (4), for, the NP absorption presents a maximum. This is so-called the Frohlich condition is associated with dipole mode .
Therefore, the strong local electric field induced by the NP (LSPR) can enhance the total electric field, and can also improve the quantum yield of the luminenescence of the RE ions from the NP (this strong enhancement of electromagnetic fields is essential in nonlinear optics effects) [64,65]. Thus, the enhancement obtained with these NPs is due to the formation of EDs which generates a polarization given by, where is the distance between each NP, is the NP specific volume, is the conduction electrons density, and e is the electronic charge . Therefore, we obtained a modification in the local electric field by these dipoles (local field correction). Using the results obtained by O.L. Malta et al , the effective electric field can be written as:
Where is the dielectric constant in the presence of an external electromagnetic field of amplitude E
Assuming that the RE ions may occupy different sites in the host, a direct coupling between the excited states of the RE ions and the NPs modifies the Stark levels energies [12,13,67]. As the NPs just give a contribution to the local field when the light is present, the oscillator strength of a spectral line, corresponding to transition from the ion ground level i to the component f of the excited level can be re-write as:
The second term into parenthesis is added to the equation from the Judd-Ofelt theory [56,57], and represents the ED transition due to LSPR of NP. To obtain non vanishing matrix elements of the components it is necessary to admix into and other states of opposite parity.
Thus, the initial and final states are:, and, then:
Where is the crystalline field, equation (16), responsible for the Stark levels and treated as a perturbation,
This can be observed experimentally in the luminescence spectra of different RE ions shown in Figure 11 interaction with silver or gold NPs in different host matrix, as a blue- or red- shift (see equation 26) and a pronounced increase in luminescence (see equation 25).
In this scenario, the influence of appeared in the luminescence spectra as a blue or a red -shift of the peaks, e.g. a transfer energy from the NPs dipoles to RE ions, thus modifying the Stark energy level’s bandwidth, see Figure 11. This energy transfer is obtained from the second term added in equation (25) and can be understood through the following definition:, where is the Racah tensor and where r
Nevertheless, an interesting question arises: how these NPs are excited?
As explained above, those NPs can be excited by a predefined incident radiation through a direct coupling between the excited states of the both RE ions and NPs, resulting in: (i) a local field increase (Frohlich condition), at
Also we can elucidate the enhancement (quenching) from the process of energy transfer as following: Er3+ emission promotes energy transfers into a plasmonic mode, which can decay nonradiatively by heat generation (Joule effect) or radiatively by releasing energy that depends on the albedo of the NPs. We consider two types of emission from a system of identical dipoles :
Where is the Rayleigh scattering [67,68] and, y = D/c, with c the speed of light. Therefore the total intensity I
We consider I
Finally, we can obtain the following conditions:, where, i.e. the luminescence enhancement depends on the incident radiation frequency and the NP size. But, as were mentioned, the incident radiation for the NP activation comes from the emitter dipole and not from the pump radiation (I
The strong local electric field induced by NPs (ED), increases the quantum yield of the RE luminescence, defined by the ratio of the local field and the incident field, , here. Thus, the maximum field enhancement is determined by the shortest distance between two equipotential particles. It corroborates well with the demonstration in the references [12,13,67,75].
Another possible mechanism for the energy transfer is due to that part of silver or gold (small silver or gold aggregates) probably remained under the form of ions, atoms, charged or neutral dimmers and multimers. Consequently, the contribution of the latter species to the RE luminescence enhancement and band shape features cannot be excluded , Figure 11. Moreover, the insertion of silver or gold in the samples leads to strong modification of the glassy network and consequently on the RE local environment, this is verified in reference .
This chapter present results where it was demonstrated the simultaneous exploitation of the enhanced local field due to NPs and energy transfer processes in order to enhance the luminescence spectra of a glassy composite material, and others. Besides, from these nanoparticles it is possible to modulate the down/up-conversion emission of the REs with applicability in areas such as optical telecommunication, including biomedical imaging and energy conversion. On the other hand, this significant enhanced fluorescence has high potential for application in photonics, optical displays, lasers and optical memory devices, amongst others. However, the success of new applications of nanoparticles depends on improvement in the understanding of the properties of LSPR and the environment around them. Further efforts and systematic studies must be realized in order to offer new developments to extend the analytical applications field of metallic nanoparticle interaction with rare-earth ions.
We hope that this chapter stimulated our readers for the development of theoretical and experimental work on plasmonics and rare-earths.
This work was financially supported by the Brazilian agencies FAPESP, CNPq and CEPOF/INOF. V.A.G. Rivera thanks to FAPESP for financial support (project 2009/08978-4 and 2011/21293-0) that allowed my pos-doctoral and my gratefully to Dr. Luiz Antonio Nunes of the Instituto de Fisica de São Carlos – University São Paulo - Brazil and the Dr. Yannick Ledemi and the Dr. Younnes Messaddeq of the Centre d'Optique, Photonique et laser – University Laval- Canada for the discussions on this issue.
Stefan Alexander Maier. Plasmonics Funadamentals and Applications. Springer Science+Business Media LLC; 2007.
Mark I. Stockman. Opt. Exp. 2011;19(22): 22029-22106.
Y. Wang, E. W. Plummer and K. Kempa. Advances in Physics 2011;60(5): 799-898.
K. Kneipp, H. Kneipp, I. Itzkan, R. R. Dasari, and M. S. Feld. J. Phys.: Condens. Matter 2002;14:R597–R624.
Y. Takeda and N. Kishimoto. Nuc. Inst. Met. Phys. Res. B 2003;206: 620–623.
Peter J. Reece. Nat. Phot. 2008;2:333-334.
Desurvire E., J. L. Zyskind and C. R. Giles. IEEE/OSA J. Ligh. Technol. 1990;LT8: 1730–1741.
A. N. Sudarkin and P. A. Demkovich. Sov. Phys. Tech. Phys. 1989;34: 764-766.
I. Avrutsky. Phys. Rev. B 2004;70: 155416-155421.
M. P. Nezhad, K. Tetz, and Y. Fainman. Opt. Express 2004;12: 4072-4079.
Chau, K. J., Dice, G. D., and Elezzabi, A. Y. Phys. Rev. Lett. 2005;94: 173904-173907.
V.A.G. Rivera, S. P. A. Osorio, Y. Ledemi, D. Manzani, Y. Messaddeq, L. A. O. Nunes, and E. Marega. Opt. Exp. 2010;18: 25321-25328.
S.P.A. Osorio, V.A.G. Rivera, L.A.O. Nunes, E. Marega, D. Manzani, Y. Messaddeq. Plasmonics 2012;7: 53-58.
V.A.G. Rivera, Y. Ledemi, S.P.A. Osorio, D. Manzani, Y. Messaddeq, L.A.O. Nunes and E. Marega. J. Non-Crys. Sol. 2012;358: 399-405.
X. Lu, M. Rycenga, S.E. Skrabalak, B.Wiley, and Y. Xia. Annu. Rev. Phys. Chem. 2009;60: 167-192.
U. Kreibig, M. Vollmer. Optical Properties of Metal Clusters. Springer-Verlag, Berlin; 1995.
Jackson John D. Classical Electrodynamics. John Wiley & Sons, Inc., New York, NY, 3rd edition; 1999.
Bohren, Craig F. and Huffman Donald R. Absorption and scattering of light by small particles. John Wiley & Sons, Inc., New York, NY, 1 edition; 1983.
Mie Gustav. Ann. Phys. 1908;25: 377-345.
E. D. Palik. Handbook of Optical Constants of Solids Academic. Elsevier, Orlando, FL. ISBN: 978-0-12-544415-6; 1985.
K. Lance Kelly, Eduardo Coronado, Lin Lin Zhao, and George C. Schatz. J. Phys. Chem. B 2003;107: 668-677.
Novotny L. and Hecht B. Principles of nano-optics, Cambridge University Press, United Kingdom, ISBN-13 968-0-521-83224-3; 2006.
Hideki Nabika and Shigehito Deki. J. Phys. Chem. B 2003;107(35): 9161-9164.
D. D. Evanoff, R. L. White and G. Chumanov. J. Phys. Chem. B 2004;108(37): 1522-1524.
H. Baida, P. Billaud, S. Marhaba, D. Christofilos, E. Cottancin, A. Crut, J. Lermé, P. Maioli, M. Pellarin, M. Broyer, N. Del Fatti, and F. Vallé. Nano Lett. 2009;9(10): 3463-3469.
C. Voisin, N. Del Fatti, D. Christofilos and F.J. Valleé. Phys. Chem. B 2001;105: 2264-2280.
F. Hache, D. Ricard and C.J. Flytzanis. J. Opt. Soc. Am. B 1986;3(12): 1647-1655.
S. Link, M. B. Mohamed and M. A. El-Sayed. J. Phys. Chem. B 1999;103: 3073-3077.
H. Kuwata, H. Tamaru, K. Esumi and K. Miyano. Appl. Phys. Lett. 2003;83: 4625-4627.
S.W. Prescott and P. Mulvaney. J. Appl. Phys. 2006;99: 123504-123510.
Cheng-ping Huang, Xiao-gang Yin, Huang Huang and Yong-yuan Zhu. Opt. Exp. 2009;17(8): 6407-6413.
Mock J. J., Barbic M., Smith D. R., Schultz D. A., and Schultz S. J. Chem. Phys. 2002;116(15): 6755–6759.
Purcell E. M. and Pennypacker C. R. Astrophys. 1973;186: 705-714.
Ruppin R. Phys. Rev. B 1982;26: 3440-3444.
Pinchuk A., Kalsin A., Kowalczuk B., Schatz G. and Grzybowski B. J. Phys. Chem. C 2007;111: 11816-11822.
Gerardy J. M. and Ausloos M. Phys. Rev. B 1982;25: 4204-4229.
Claro F. Phys. Rev. B 1984;30: 4989-4999.
Rojas R. and Claro F. Phys. Rev. B 1986;34: 3730-3736.
Olivares I., Rojas R., Claro F. Phys. Rev. B 1987;35: 2453-2455.
M. Chergui, A. Melikian , H. Minassian. J. Phys. Chem. C 2009;113: 6463–6471.
P. P. Sorokin and M. J. Stevenson. Phys. Rev. Lett. 1960;5: 557-559.
D.C. Brown. IEEE J. Sel. Top. Quantum Electron. 2005;11: 587-599.
S. Hufner. Optical Spectra of Transparent Rare Earth Compounds. Academic press New York – San Francisco – London; 1978.
B.R. Judd. Operator Techniques in Atomic Spectroscopy. McGraw-Hill, New York; 1963.
B.G. Wybourne. Spectroscopic properties of Rare Earths, Wiley, New York; 1965.
A.J. Freeman and R.E. Watson. Phys. Rev. 1962;127: 2058-2075.
A.J. Kenyon. Prog. Quan. Elec. 2002;26: 225–284
Michel J.F. Digonnet and Marcel Dekker. Rare-earth-doped fiber lasers and amplifiers. 2d ed., edited by, Inc. New York – Basel; 2001.
V.A.G. Rivera, E.F. Chillce, E.G. Rodrigues, C.L. Cesar, L.C. Barbosa. J. Non-Crys. Sol. 2006;353: 125-130.
V.A.G. Rivera, E.F. Chillce, E.G. Rodrigues, C.L. Cesar, L.C. Barbosa. Proc. SPIE 2006;6116: 190-193.
P.J. Mears, L. Reekie, I.M. Jauncey and D.N. Payne. Elec. Lett. 1987;23: 1026-1028.
E. Desurvire, R.J. Simpson and P.C. Becker. Opt. Lett. 1987;12: 888-890.
E. Desurvire. Phys. Today 1994;47: 20-27.
M. Yamane and Y. Asahara. Glasses for Photonics. Cambridge - University Press, Cambridge, United Kingdom; 2002.
J.H. van Vleck. J. Phys. Chem. 1937;41: 67-80.
B.R. Judd. Phys. Rev. 1962;127: 750-761.
G. S. Ofelt. J. Chem. Phys. 1962;37: 511-520.
Arai K., H. Namikawa, K. Kumata, T. Honda, Y. Ishii, T. Handa. J. Appl. Phys. 1986;59: 3430–3436.
Shimizu M., M. Yamada, M. Horigucho and E. Sugita. IEEE Pho. Tech. Lett. 1990;2: 43–45.
V.A. Markel, V. M. Shalaev, E. B. Stechel, W. Kim, and R. L. Armstrong, Phys. Rev. B 1996;53: 2425.
V. M. Shalaev, E. Y. Poliakov and V. A. Markel. Phys. Rev. B 1996;53: 2425-2449.
V.A.G. Rivera, S.P.A. Osorio, D. Manzani, Y. Messaddeq, L.A.O. Nunes, E. Marega Jr. Opt. Mat. 2011;33: 888-892.
N. M. Lawandy. Appl. Phys. Lett. 2004;85: 5040-5042.
S. Kim, J. Jin, Y. Kim, I. Park and Y. Kim. Nature 2008;453: 757-760.
S. Kuhn, U. Hakanson, L. Rogobete and V. Sandoghdar. Phys. Rev. Lett. 2006;97: 017402.
O.L. Malta, P.O. Santa-Cruz, G.F. de Sá and F. Auzel. J. of Lumin. 1985;33: 261-272.
T. Som and B. Karmakar. J. Appl. Phys. 2009;105: 013102.
L.R.P. Kassab, F.A.Bonfim, J.R. Martinelli, N.U. Wetter, J.J.Neto and Cid B. Araujo. Appl. Phys. B 2009;94: 239-242.
T. Som and B. karmakar. J. Opt. Soc. Am. B 2009;26(12): B21-B27.
Krishna Kanta Haldar and Amitava Patra. App. Phys. Lett. 2009;95: 063103.
Thiago A. A. Assumpção, Davinson M. da Silva, Luciana R. P. Kassab and Cid B. de Araújo. J. App. Phys. 2009;106: 063522.
Maik Eichelbaum and Klaus Rademann. Adv. Funct. Mater. 2009;19: 2045–2052.
A. Gopinath, S. V. Boriskina, S. Yerci, R. Li and L. Dal Negro. Appl. Phys. Lett. 2010;96: 071113.
J. R. Lakowicz. Anal. Biochem. 2005;337: 171-194.
F. Le, D. W. Brandl, Y. A. Urzhumov, H. Wang, J. Kundu, N. J. Halas, J. Aizpurua, and P. Nordlander. ACS Nano 2008;2: 707-718.
- A SPP is an electromagnetic wave propagating along the interface between two media possessing permittivities with opposite signs, such as the metal–dielectric interface.
- Localized surface plasmons have been observed since the Romans who used gold and silver nanoparticles to create colored glass objects such as the Lycurgus Cup (4th Century A.D.). A gold sol in the British museum, created by Michael Faraday in 1857, is still exhibiting its red color due to the plasmon resonance at ,530 nm [L. M. Liz-Marzan, Mater. Today 7, 26 (2004).].