Open access peer-reviewed chapter

Nanoplasmonic Waveguides Filled with Electro‐Optical Materials

Written By

Montasir Qasymeh

Submitted: 08 September 2016 Reviewed: 28 December 2016 Published: 21 June 2017

DOI: 10.5772/67370

From the Edited Volume

Nanoplasmonics - Fundamentals and Applications

Edited by Gregory Barbillon

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In this chapter, nanoplasmonic waveguides filled with electro-optical materials are proposed and discussed. Rigorous theoretical modelling is developed to describe the propagation, generation and control of electromagnetic fields confined in these nanoscale waveguides. Two configurations are studied thoroughly. First, a metal-insulator-metal (MIM) nanoplasmonic waveguide filled with lithium niobate (i.e., LiNbO3) is considered for compact terahertz (THz) generation. The waveguide is designed to generate Gaussian THz waves by the means of frequency down-conversion of two surface plasmon polariton (i.e., SPP) modes. THz generation is shown to be viable over the entire range from 1 to 10 THz by properly designing the SPP wavelengths and waveguide dimensions. Future applications of such nanoscale THz sources include nanocommunication systems and body-centric networks. Secondly, an MIM nanoplasmonic waveguide filled with doped LiNbO3 is considered. The interaction between two interfering SPP modes is studied. It is shown that a strong symmetric SPP mode can be coupled to a weak antisymmetric SPP mode by the means of photorefractive effect. Future advances include implementing known photorefractive applications (such as interferometry and holography) in the nanoplasmonic field. The work of this chapter highlights the potential of functioning electro-optical materials in nanoplasmonic waveguides to achieve novel ultra-compact and efficient devices.


  • plasmonic waveguides
  • electro‐optic material
  • lithium niobate
  • terahertz
  • photorefractive effect

1. Introduction

Nanoplasmonic waveguides offer unprecedented tight confinement of electromagnetic waves in subwavelength structures. In principle, nanoplasmonic waveguides comprise several metal‐dielectric layers. The propagating light is coupled to the free electrons in the metal, which acts like plasma at the optical frequency. It then follows that the propagating light can be strongly confined even to 100 times smaller than its wavelength. Such tight confinement has the potential to open a new world of scalability and integration. For instance, nanoplasmonic‐based devices can be utilized as matching interconnectors between traditional micro‐photonics and nanoelectronic devices [15]. This paves the way for the development of efficient, compatible and ultrafast chips [68]. However, the achievable tight confinement in the nanoplasmonic waveguides can be functioned to boost the propagating waves’ intensities. It then follows that the nonlinear effects can be significantly enhanced, and thus, desired functionalities can be achieved. To date, several advances in plasmonic technology have been reported. These include all optical nanoplasmonic logic gates [9], electrically controlled plasmonic devices [10], plasmonic amplification and lasing [11], efficient second harmonic generation using plasmonic waveguides [12], silicon‐on‐insulator‐compatible plasmonic devices [13], focus and enhancement of terahertz (THz) radiation using plasmonic waveguides [14], efficient and ultra‐compact hybrid plasmonic devices [15], solitonic plasmonic waveguides [16] and mode conversion in plasmonic waveguides [17], to mention a few examples.

In this chapter, nanoplasmonic waveguides filled with electro‐optical materials are proposed and discussed. Specifically, metal‐insulator‐metal (MIM) plasmonic waveguides filled with lithium niobate (LiNbO3) are considered. The theoretical models that describe the nonlinear interaction of the confined electromagnetic waves in nanoplasmonic waveguides are developed. Numerical evaluations based on experimentally reported parameters are provided. Two different configurations are studied thoroughly. The first configuration is a MIM nanoplasmonic waveguide designed for compact THz generation [18]. The optical pumps are guided by means of surface plasmon polaritons (SPPs), whereas the generated THz waves are designed to diffract and propagate outside the MIM waveguide. The design of this work attains the following desired properties: first, the THz absorption is minimized. Secondly, the proposed structure is compact and relevant for nanoapplications. Thirdly, the generation efficiency is maximized by reducing losses rather than introducing resonant conditions (i.e. phase matching), and thus, wide THz generation is achieved. We note that this proposal introduces a new modality from the standpoint of applications. For instance, the proposed MIM nanostructure can be immersed inside a target (such as a cell or a biological entity), and the generated THz waves can interact with the (under‐test) surrounding medium of the MIM nanostructure, while the optical modes are tightly confined inside the MIM nanostructure. Potential future applications include nanocommunication networks and body‐centric systems. The second configuration considered in this work includes MIM plasmonic waveguide filled with doped LiNbO3 [19]. The main interest is to study the interaction of the interfering SPP modes with the doping impurities. To model the interaction analytically, small intensity modulation interference depth is considered and a perturbation approach is employed. The evolution of the interfering modes is obtained to quantify the interaction. On considering strong pump and weak signal scenario, it is found that the two SPP modes are coupled by means of the photorefractive effect. The modal gain is calculated to characterize the photorefractive effect. First, an ideal case of lossless waveguides is considered, and the gain versus the waveguide length, the doping concentration and the input amplitudes are characterized. Secondly, the modal losses are taken into account. It is found that a weak antisymmetric mode can experience an effect gain up to certain waveguide lengths in the presence of a strong symmetric mode, considering proper doping concentration and input amplitudes. The coupling effect can be conceived either as an amplification or mode‐conversion process, promising novel future application.

The remaining part of this chapter is organized as follows. The propagation modes and the dispersion relation of MIM plasmonic waveguides are introduced in Section 2. The nonlinear and the electro‐optical coefficients of the LiNbO3 are introduced in Section 3. THz generation in nanoplasmonic waveguides is discussed in Section 4. The photorefractive effect in nanoplasmonic waveguides is discussed in Section 5. Finally, concluding remarks are presented in Section 6.


2. MIM Plasmonic waveguides

Consider an MIM plasmonic waveguide comprising two metallic layers sandwiching a LiNbO3 of thickness a, as depicted in Figure 1. The waveguide is two dimensional and independent of the y‐axis.

Figure 1.

The MIM plasmonic waveguide filled with LiNbO3. The spatial distribution of electric field x component is schematically displayed, in red, for both the symmetric and antisymmetric modes.

The waveguide has two fundamental propagating SPP modes of symmetric and antisymmetric transverse field distribution at specific frequency ω, classified according to the spatial distribution of the x electric field component. The expression of the electric field associated with the symmetric and antisymmetric modes, i.e. Es  and Ea, are given by [20]:


where As (and Aa) and βs (and βa ) are the complex amplitude and propagation constant of the symmetric (and antisymmetric) propagating mode, respectively, j=1, c.c. is the complex conjugate and D(z) and v(z) are the spatial distributions, given by [20].


Here, a2<z<a2, εx,z is the LiNbO3 relative permittivity for x and z polarization, respectively, and kcs(a)=εzεxβs(a)2εzk02 is the core transverse decay factor for the symmetric (and antisymmetric) SPP mode.

On applying the boundary conditions, the dispersion relation for the symmetric and antisymmetric modes can be, respectively, given by the following [20]:


where kms(a)=βs(a)2εmk02 is the transverse decay factor in the metal for symmetric (antisymmetric) SPP mode, k0=2πλ is the propagation constant in the free space, and εm is the metal permittivity.

One may rewrite the dispersion relation in the following form [18]:


The dispersion form in Eq. (4) can be solved numerically for kc, for a known frequency ω and slot thickness a. The propagation constant β can then be calculated by βs,a2=εxεzkcs,a2+εxk02.


3. LiNbO3 coefficients

LiNbO3 is chosen as the electro‐optical material for this work. Consider the indices of the LiNbO3 (1, 2, 3) along the axes (x, y, z ), respectively. Given that the MIM waveguide is independent of the yaxis, the propagating fields have x and z electric field components, denoted by Ex and Ez. The nonlinear polarization induced in the LiNbO3 is given by the following [21]:


where PNLJ is the Jth nonlinear polarization component and d22=3 pm/v, d31=5 pm/v, and d33=33 pm/v are the nonlinear coefficients. Several phenomena are attributed to the nonlinear polarization, including new frequency generation, frequency conversion and polarization rotation, to mention a few. The evolution of the propagating fields is governed by the nonlinear wave equation that involves the nonlinear polarization. An example of THz generation based on induced nonlinear polarization in MIM nanoplasmonic waveguide is discussed in the next section.

The electro‐optic coefficients are related to the nonlinear coefficients by the following:


where nx and nz are the principal refractive indices.

The effective permittivity of the LiNbO3 depends on the electric field components, by means of electro‐optic effect, through the following relation [21]:


where εeff is the effective permittivity of the LiNbO3 and ε is the intrinsic permittivity of the LiNbO3.

On considering a small induced change in the permittivity, so that (r15r22)Ex+r13Ex1εx and r15Ex+r33Ex1εz, the effective permittivity can be approximated by the following [19]:


In Section 5, an example of photorefractive effect in MIM plasmonic waveguide based on the electro‐optic effect is discussed.


4. THz generation in nanoplasmonic waveguides

In this section, an MIM plasmonic waveguide filled with LiNbO3 and with two propagating SPP modes is considered. The frequency difference between the two SPP modes is properly designed for THz generation. Theoretical modelling and numerical evaluations are presented.

4.1. Field expressions

As the symmetric mode is a fundamental mode of the MIM waveguides, two symmetric modes with distinct frequencies ω1 and ω2 are considered for this work. It then follows that a single mode at each specific frequency can be propagated given a proper waveguide thickness a. The associated electric fields have x and z polarization components, given by the following:


Here i{1,2}.

The THz wave is generated by means of difference‐frequency generation of the two SPP modes enabled by the LiNbO3 nonlinearity.

The MIM structure is designed to guide the SPP pumps, whereas the generated THz waves are designed to diffract and propagate outside the MIM waveguide, as shown in Figure 2. The thickness of the metallic layer is equal to d=5km. It then follows that 99% of the optical SPP modes are confined inside the MIM waveguide, and thus one may conceive the metallic layers to be of infinite thickness. However, because THz waves are of wavelengths much greater than the MIM waveguide dimension, and given that THz waves cannot be guided as SPP modes [22], the generated THz waves will diffract into the surrounding medium and evolve as a Gaussian beam. The generated THz waves can be modelled as a transverse electromagnetic (TEM) Gaussian beam, given by [23] and [24]:


Figure 2.

The MIM plasmonic waveguide for THz generation.

where G(x)=(2/π)14W0γ(z)exp(x2γ(z)W02),ATHz is the complex amplitude, W0 is the beam spot at z=0, γ(z)=1+jz/ZR, and ZR is the Ray Leigh rang given by W02πλ.

4.2. Nonlinear polarization

The induced nonlinear polarization components are at the frequencies ω1, ω2, ω1ω2, and ω1+ω2. Here, the frequency difference between the two optical frequencies ω1 and ω2 is designed to lie in the THz range. It must be noted that this generated THz wave at ω1ω2 cannot be guided by the plasmonic MIM waveguide [22], as previously mentioned. The other generated harmonic at ω1+ω2 lies in the optical frequency range, close to the second harmonic frequency, and is guided as SPP mode [25]. It then follows that the wave at ω1+ω2 suffers from strong attenuation. Thus, the nonlinear polarization component at frequency ω1+ω2 will be ignored in the following analysis. On the substitution of the fields of Eqs. (9) and (10) into Eq. (5), the nonlinear polarization components can be obtained. The nonlinear polarization components at ω1 are as follows:


the nonlinear polarization components at ω2 are


and the nonlinear polarization component at ωTHz=ω1ω2 is


The zcomponent of the nonlinear polarization at ωTHz is not considered because the generated THz wave is a TEM Gaussian wave that propagates in the z direction. Therefore, the THz wave has a zero zcomponent electric field. In other words, the xcomponent of the nonlinear polarization, i.e. PNLx, is the only source that contributes to the evolution of the generated THz wave.

4.3. THz generation

The evolution of the generated THz wave and the SPP modes are governed by the nonlinear wave equation, given by:


On the substitution of the fields of Eqs. (9) and (10) into Eq. (14), and using the nonlinear polarization expressions of Eqs. (1113), the corresponding slowly varying envelope approximation (SVEA) equations can be formed, given by the following [18]:


where ϕ/δ=a2+a2ϕ*(ζ)δ(ζ)ζ.

The evolution of the THz and the SPP fields can be obtained by numerically solving the SVEA Eqs. (1517). However, various losses must first be precisely evaluated. These include SPP and THz losses. The decay factor of the SPP linear losses can be calculated from the imaginary part of the propagation constant, i.e. αLi=Im{βi}, by solving Eq. (4). These SPP linear losses can be taken into account by incorporating the corresponding decay factor αLi in the SVEA Eqs. (15) and (16). The SPP nonlinear losses are described by the decay factor αNL, given by αNL=γNL.I [26]. Here, γNL=2.7×105 m/W is the nonlinear absorption coefficient of LiNbO3 crystal, and I is the power of the SPP modes. Our investigations show that the nonlinear losses in this work are much smaller than the linear losses, and can be ignored despite the large SPP intensities because the waveguide lengths considered in this work are very small and lie in the micro‐meter range. However, the THz losses are also mainly linear, given the low generated intensities. The effective decay factor of the THz losses is given by the following:


where αTHzMetal is the metal THz absorption coefficient, αTHzLN is the LiNbO3 THz absorption coefficient and W is the Gaussian beam spot given by W=W01+(zzR)2. To take the THz losses into account, one must incorporate the effective THz decay factor of Eq. (18) into the SVEA Eq. (17). Experimental values of metal and LiNbO3 absorption coefficients can be found in the literature. For example, in [27] the absorption coefficient of gold is given by αTHzMetal=6×106 m1, and in [28] the absorption coefficient of the LiNbO3 is given by αTHzLN=2×104 m1, both for the 4 THz frequency. It must be noted that the total THz losses are minimized in this work, as can be inferred from Eq. (18). This is because the generated THz waves diffract rapidly to propagate outside of the MIM plasmonic waveguide even for a few 10's of nanometers of propagation. For instance, considering a 4 THz wave, the beam spot evolves from 120 nm (which is the slot thickness, i.e. a ) to approximately 10 μm by propagating only 50 nanometers.

4.4. Numerical evaluations

In the following analysis, we consider gold for the two metallic layers, a slot thickness of a=120 nm, a metal thickness of d=110 nm and As1(0)=As2(0)=1 V/μm. In Figure 3, the power of a 4 THz generated wave is shown versus the waveguide length. Here, λ1=1550 nm and λ2=1582 nm. The power is calculated per unit width, defined by pi=12ε0cni|Asi|2+vivi*x and pTHz=12ε0cnTHz|ATHz|2GG*x, where the SPP power is p1+p2.

Figure 3.

Power of the generated 4 THz wave, and SPPs power versus waveguide length.

As can be seen in Figure 3, the effective waveguide length is limited to 35 μm and most of the SPP power is dissipated by losses.

The optics‐to‐THz conversion efficiency can be defined as η=pTHz(L)p1(0)+p2(0), where pTHz(L) is the THz power per unit width, L is the MIM waveguide length, and p1,2(0) is the input SPP powers per unit width.

In Figure 4, the conversion efficiency for a 4 THz generated wave is presented versus the input SPP power. Here, we consider a waveguide length of L=35 μm, λ1=1550 nm and λ2=1582 nm. Additionally, a hypothetical case of phase‐matched generation is presented (by setting β1β2βTHz=0) for comparison. As can be seen, the phase‐matching enhancement is maximally approximately 4 THz because the interaction is limited by losses. For instance, for 4 THz generation and λ1=1550 nm, the beat length LB(defined by LB=2πβs1βs2βTHZ) is approximately 42 μm, whereas the SPP propagation length (defined by LSPP=(2α)1) is approximately 25 μm. Thus, it is intuitive to expect limited enhancement of phase‐matched operation.

Figure 4.

Conversion efficiency for a 4 THz wave versus total SPP input power. The two scenarios of phase matching and phase mismatching are shown for comparison.

The frequency of the generated THz wave can be tuned by controlling the frequency difference between the two SPP modes, i.e. f1f2. In Figure 5, the wavelength 1 is fixed at λ1=1550 nm, whereas wavelength 2 is tuned to generate different THz wave frequencies from 1 to 10 THz. As can be seen from Figure 5, THz waves can be generated over the entire range from 1 to 10 THz simply by tuning the frequency ω2. Furthermore, different slot waveguide thicknesses are considered in Figure 5. These include a= 75, a=120 and a=185 nm. It can be seen that, for the same SPP input, smaller slot thickness result in weaker generated THz waves. This is due to higher losses for smaller slot thickness. Thus, as expected, more compact generation is achieved at the cost of higher losses.

Figure 5.

Power of the generated THz wave versus its frequency. Different slot thicknesses are considered. The optical wavelength λ1 is fixed at the value λ1=1550 nm. The waveguide length is L=35 μm.


5. Photorefractive effect in nanoplasmonic waveguides

In this section, the LiNbO3 filling the MIM waveguide is doped with ND donor and NA acceptor atom impurities. The interaction between two (symmetric and antisymmetric) interfering SPP modes is studied.

5.1. Intensity expression

The electric fields of the two symmetric and antisymmetric propagating modes are described by Eq. (1). The optical field intensity inside of the waveguide, I=(Es+Ea)(Es*+Ea*), can be formed as follows:


where Δβ=βaβs, Io(x,z)=T1(x)|Aa(z)|2+T2(x)|As(z)|2, I1(x,z)=T3(x) Aa(z) As*(z), T1(x)=Dx(x) Dx*(x)+Dz(x) Dz*(x), T2(x)=vx(x) vx*(x)+vz(x) vz*(x), and T3(x)=2Dx(x) vx(x)+2Dz(x) vz(x).

On adapting a strong pump and weak signal scenario, i.e. I1I0, a perturbation approach can be implemented to model the evolution of the propagating fields.

5.2. Band transport model

The interaction of the interfering SPP modes with LiNbO3 impurities is governed by the standard band transport model that encompasses the electron continuity equation, the current density equation and the Poisson's equation, as in the following [29]:


where N is the free electron density, NDi is the ionized donor density, e is the electron charge, J=eNμESC+kBTμN+κ(NDNDi)sIe^z is the conduction current density, μ is the LiNbO3 electron mobility, kB is the Boltzmann constant, T is the temperature, κ is the photovoltaic constant, ESC is the space charge electric field, and ε is the LiNbO3 permittivity. The three coupled equations of the band transport model shown above can be solved analytically by obeying a perturbation approach for a small depth intensity modulation limit i.e. I0  I1. Towards solving these three coupled equations (20)(22) for a continuous wave case, and considering small intensity modulation, the electron density N and the ionized donor density NDi can be written in the following form:


where N0 and ND0i are the averages of electron and ionized donor densities, and N1 and ND1i are the modulation amplitudes of electron and ionized donor densities, respectively.

The space charge electric field ESC can be uniquely specified through Eq. (22) and the electrostatic condition, i.e. ×ESC=0.

Consequently, on substituting Eq. (23) into Eq. (22), and using the electrostatic condition, one can obtain the following expression [19]:


Where cSC=ejΔβε0εx(kcs+kca)2+ε0εz(jΔβ)2

By substituting Eq. (23) into Eqs. (20) and (21), and considering a steady state so that the time rates of the free electrons and the ionized donor densities are zeros (i.e. Nt=NDit=0) [29], the expressions for N0, ND0i, N1 and ND1i can be obtained. First, by substituting Eq. (23) in Eqs. (20) and (21), equating the average terms, and using N0+NAND0i=0, one obtains the following:


Secondly, by substituting Eq. (23) into Eqs. (20) and (21) and equating the modulation terms (i.e. those with eiΔβz ), one obtains:


where a1=s(NDND0i), a2=N0γR+SI0, a3=ND0iγR, b1=μ((kcs+kca)2+(jΔβ)2)×(kBTe2N0ε0εx(kcs+kca)2ε0εz(jΔβ)2), b2=κs(jΔβ)2+e2N0μ((kcs+kca)2+(jΔβ)2)ε0εx(kcs+kca)2ε0εz(jΔβ)2 and b3=κs(NDND0i)(jΔβ).

The spatial electric field ESC can be evaluated by performing the following three steps. First, one must calculate the average electron and ionized donor densities, i.e. N0 and ND0i, using Eqs. (25) and (26). Secondly, the modulation amplitudes of electron and ionized donor densities, i.e. N1 and ND1i, can be calculated using Eqs. (27) and (28). Finally, the ESC can be evaluated by using Eq. (24). The spatial electric field modifies the effective permittivity of the MIM waveguide, by means of electro‐optic effect, causing the SPP modes to be coupled in a phase‐matched fashion, a phenomenon known as the photorefractive effect.

5.3. Photorefractive effect

The evolution of the SPP modes are governed by nonlinear wave equation, given by:


where D is the displacement current given by D=ε0εeffE.

The effective permittivity can be obtained by substituting the spatial electric field, i.e. ESC, of Eq. (24) into Eq. (8), yielding the following:


where εx1=(εx)2(r13csc(N1ND1i)+(r15r22)cscjΔβ(N1ND1i)x), and εz1=(εz)2(r33csc(N1ND1i)+r15cscjΔβ(N1ND1i)x)

On the substitution of symmetric and antisymmetric mode expressions of Eq. (1) into Eq. (29) and using Eq. (30), the fields equations (for slowly varying amplitudes) can be obtained, given by the following [19]:


Where c1=2eΔβε0εx(kcs+kca)2+ε0εz(jΔβ)2(N1I1ND1iI1)(βaβs(ωε0εx)2kcskca(ωε0εz)2),

As can be seen in Eqs. (31) and (32), the two SPP modes are coupled in a phase‐matched fashion. The coupling is conducted by the spatial space charge electric field generated by the interfering SPP modes in the doped LiNbO3. This is known as the photorefractive effect. The photorefractive effect has been known since the early 1960s [30] in bulk materials and micro‐meter dielectric waveguides. In this work, the photorefractive effect is investigated in nanoplasmonic waveguides. Numerical evaluations are presented in the following section.

5.4. Numerical evaluations

To illustrate the potential of the photorefractive effect in plasmonic waveguides, typical realistic values are considered. Consider r13=11 pm/V, r33=34 pm/V, T=300K, μ=7.4×105m2/(V.s), S=2.34×108m2/(s.V2), κ=1.5×1011(m/V) and γR=2.4×1013m3/s [29, 31, 32]. In this work, the blue wavelength λ=458 nm is considered, given its known functionality in photorefractive devices. The LiNbO3 permittivity is εz=5.177 and εx=5.624 at this wavelength. Also, the aluminium metal (i.e. Al) is chosen as the cladding material, that has a permittivity of εm=29+7j at λ=458nm.

First, the waveguide losses are ignored and the gain versus the doping concentration and the input amplitudes is characterized. Different slot thicknesses are considered. Secondly, the modal losses are taken into account, considering proper doping concentration and input amplitudes.

Our numerical investigations show that gain can be realized only for weak antisymmetric mode (the signal) co‐propagating with strong symmetric mode (the pump). This is because the space charge electric field, that couples the two modes, has an antisymmetric transverse distribution, as can be inferred from Eqs. (2), (19) and (24).

In Figure 6, the antisymmetric gain, defined by Aa(L)/Aa(0), is displayed versus the waveguide length L in (a), the doping concentration ND in (b), the inputs ratio Aa(0)/As(0) in (c) and the input pump amplitude As(0) in (d). The modal losses are ignored and three different thicknesses (i.e. a=50 nm, a=70 nm and a=90 nm) are considered. In (a), |Aa(0)|=0.001×|As(0)| and ND=12×1020m3. In (b), the waveguide length L=84 μm, |As(0)|=1.935×103(V/m), and |Aa(0)|=0.001×|As(0)|. In (c), the waveguide length L=84 nm, ND=12×1020m3. In (d), the waveguide length L=84 nm, ND=12×1020m3 and Aa(0)/As(0)=103.

Figure 6.

The antisymmetric gain (a) versus waveguide length; (b) versus the doping concentration ND; (c) versus the input ratio Aa(0)As(0); and (d) versus the input pump field amplitude As(0).

As can be seen from the simulations in Figure 6, the photorefractive response, characterized by the gain, is qualitatively the same for different waveguide thicknesses, given losses are ignored. However, it can be seen from part (b) that the gain crucially depends on the doping concentration; the stronger the effect, the larger the doping concentration. Furthermore, it can be seen from part (c) that the gain does not dramatically depend on the input ratio, given that the perturbation condition is satisfied, i.e. A(0)a/A(0)s1. Finally, it can be seen from part (d) that the gain is crucially depending on the pump input amplitude (i.e. the symmetric mode input amplitude); the stronger the effect, the larger the input amplitude. These properties characterize the photorefractive effect considering ignored losses. Same properties are expected for fields propagating few micrometers of waveguide length. However, for larger waveguide lengths, such as 10's or 100's of micro‐meters, altered characteristics are expected, given that losses are dominating for such waveguide length ranges [19].

Losses can be taken into account by incorporating the effective decay factor, given by αeffs,a=Im{βs,a}, in Eqs. (31) and (32).

In Figure 7, the antisymmetric gain is presented against the waveguide length. Here, losses are taken into account. Three different thicknesses of a=50 nm, a=70 nm and a=90 nm are considered with input pump amplitudes of 4.7×103(V/m), 16.5×103(V/m), and 18.4×103(V/m) are presumed, respectively. The input pump amplitudes are chosen so that the maximum gain is identical for the three thicknesses for the purpose of comparison. As can be seen in Figure 7, a significant gain can be experienced despite losses with the maximum gain attainable at the same waveguide length L=1.1 μm. However, a net gain is experienced up to different waveguide lengths for different thicknesses. This is because the photorefractive effect dominates the interaction for the first few micro‐meters, whereas losses limit the interaction for larger waveguide lengths, with greater antisymmetric losses for larger waveguide thicknesses.

Figure 7.

The antisymmetric gain versus waveguide length, for three different LiNbO3 thicknesses, taking losses into account.

Figure 8 depicts the results of Figure 7 in dB units. As can be seen, given the assumed parameters, the maximum achieved gain can be 28.8 dB for the three different thicknesses. It can also be seen that for different waveguide thicknesses, the photorefractive gain compensate losses up to different waveguide lengths. For instance, the zero dB gain can be achieved at waveguide lengths of L=41 μm, L=16.2 μm and L=10.6 μm for waveguide thicknesses of a=50 nm, a=70 nm and a=90 nm, respectively, for the same reason mentioned above explained by having greater antisymmetric losses for larger waveguide thicknesses.

Figure 8.

The antisymmetric gain in dB versus waveguide length, taking losses into account.


6. Conclusion

Nanoplasmonic waveguides filled with electro‐optical material were proposed and discussed. The aim of this work is to incorporate the unique properties of plasmonic waveguides, ultra‐compact structures and high internal intensities, with electro‐optical material properties, thus achieving novel functionalities. Two configurations were chosen and investigated. First, an Au‐LiNbO3‐Au nanostructure waveguide is considered for THz generation by means of difference‐frequency generation of SPP modes. The SPP modes are designed to be totally confined inside the waveguide, whereas the generated THz waves are concentric with the SSP modes and contained mainly in the surrounding medium of the waveguide. Several advantages are achieved through this design. First, THz losses are minimized. Secondly, an off‐resonance operation is conducted. Finally, a nanoscale and yet simple THz generation is offered. The evolution of the THz wave and the SPP modes are evaluated and found to be mainly limited by losses. Nevertheless, THz generation is shown to be viable over the entire range from 1 to 10 THz by properly designing the SPP wavelengths and waveguide dimension. Possible future applications include nanocommunication systems and body‐centric networks. Secondly, an AL‐LiNbO3‐AL nanostructure is considered with the LiNbO3 being doped with donor and acceptor atom impurities. Two SPP modes with symmetric and antisymmetric spatial distribution are considered. The interaction of the interfering SPP modes with the atom impurities is modelled. It was found that the SPP modes are coupled by the means of the photorefractive effect. A net gain was shown viable for weak antisymmetric mode co‐propagating with strong symmetric mode. The antisymmetric gain was studied against the doping concentration and the input amplitudes. This work opens up new opportunities to apply known photorefractive applications to nanoplasmonic devices. The two configurations discussed in this chapter demonstrate the potential of utilizing electro‐optical materials in nanoplasmonic waveguides to achieve novel, efficient and ultra‐compact devices.



This work was supported by the Centre on Smart Service for Smart Cities at Abu Dhabi University, UAE, under grant 19300066.


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Written By

Montasir Qasymeh

Submitted: 08 September 2016 Reviewed: 28 December 2016 Published: 21 June 2017