Tunable Unidirectivity of Metal-Dielectric-Metal Plasmonic Nanoantennas With PT-Symmetric Potentials

Introduction

Surface plasmon polaritons (SPPs) refer to collective oscillations of conductive electrons at metal and dielectric interface [1]. With metallic nanostructures at the interface, these excitations couple strongly with light, giving rise to large interaction cross-sections, and enhanced near-fields [2, 3]. When the optical field couples with the SPPs in plasmonic nanostructures, some fascinating features, and applications arise, such as photo-thermal cancer therapy [4], ultra-sensitive bio-sensing [5], and improved solar energy harvesting [6], etc. However, it is well known that the intrinsic absorption of plasmonic nanostructures is usually high, especially at optical frequency, resulting in low performance efficiency [7]. Intrinsic absorption of the metallic nanostructures [8–11] can be substantially reduced with the assistance of active materials such as dye molecules, rare earth ions, or semiconductor crystals [3]. This is because the active materials can give rise to lasing or field amplification under external pumping, and transfer energy to compensate the losses of the SPPs [12–15]. Consequently, active materials enable the development of novel light-emitting devices [16, 17], such as spasers [18–20] or, more generally, plasmonic nanolasers [21–27]. It is also important to note that tuning the level of gain shall pave a path to dynamically control the response of these systems [3, 28, 29].

Recently, a new wave of interest in active materials appears in the realm of PT-symmetric systems [3, 30]. A system with PT-symmetry is comprised of active and absorptive elements which are in appropriate spatial distribution, such that the system presents a balanced gain and loss. PT-symmetry condition is directly translated into a requirement for the dielectric function of the system, ε(r) = ε*(−r), which can be achieved using active elements [3, 31, 32]. In other words, to achieve a PT-symmetric optical potential, the real part of the permittivity shall be an even function of position while its imaginary part must be an odd one. The interest in PT-symmetry of photonic systems relies on the exotic properties including, to cite some [3], asymmetric propagation [33, 34], reflection [35], scattering [36], unidirectional invisibility [37, 38], switching [39, 40], and extraordinary non-linear behaviors [41, 42]. These intriguing phenomena have been already observed in dielectric waveguides [43] and cavities [44] or photonic lattices [45, 46], among other realizations [3].

In this regard, plasmonic nanostructures with PT-symmetry have been attracting increased attention. A pioneer study has shown that the strong interaction of surface plasmons with light can be exploited to enhance the extraordinary properties arising from the PT-symmetry [3, 47]. Successive works demonstrate asymmetric behaviors in waveguides [48] and metamaterials [49, 50], transition from absorption to amplification in cavities [51] and waveguides [52], unidirectional cloaking [53], switching [54], multiplexing [55], anisotropic emission in hybrid nanoparticles [56], and giant near-field radiative heat transfer [3, 57].

In this paper, we investigate asymmetric optical response of a plasmonic nanoantenna that operates near the PT-symmetry condition. The nanoantenna is stacked with three metallic blocks and two dielectric blocks. Each of the two dielectric blocks, sandwiched by metallic ones, is either absorptive or active, respectively, with the same value of κ but in opposite sign. With such a PT-symmetric configuration, the antenna supports a highly tunable magnetic dipole (MD) that spectrally overlaps an electric dipole (ED) mode. And the tunability is primarily dependent on the variation of κ. It is also interesting to note that the interference between the MD and ED modes gives rise to superior unidirectional scattering. The side lobe level, of forward and backward radiation, can be suppressed in the cases provided that the Kerker conditions are well-satisfied. Furthermore, we show that the scattering direction of the nanoantenna strongly depends on the non-Hermiticity parameter κ. In particular, it is feasible to switch the scattering direction of the antenna at the same wavelength in a wide spectra band by adjusting κ. We also find that the beam-width of the scattered light can be further narrowed when the antenna multilayers are arranged in a chain.

Materials and Methods

For The scattered far-field for homogeneous and substrate environments can be written as [58],

$\begin{array}{l}{\text{E}}_{\text{SC}}^{0,\text{ FF}}(\text{r})\simeq {\omega }^2{\mu }_0\frac{e^{i{k}_{\text{d}}(r-\text{n}·{\text{r}}_0)}}{4\pi r}[\text{n}\times (\text{p}\times \text{n})-\frac{1}{v_{\text{d}}}(\text{n}\times \text{m})\\ +\frac{i{k}_{\text{d}}}{6}[\text{n}\times (\text{n}\times Q^e\text{n})]\\ +\frac{i{k}_{\text{d}}}{2v_{\text{d}}}(\text{n}\times Q^m\text{n})+\text{n}\times (\frac{i{k}_{\text{d}}}{v_{\text{d}}}\text{T}\times \text{n})]& (1)\end{array}$

where ω is the angular frequency, r is the spatial coordinate vector, μ₀ = 4π·10⁻⁷ H/m is the vacuum permeability, v_d = c(ε_d)^−1/2, c is the speed of light in vacuum, ε_d is the relative permittivity of dielectric surrounding, r = |r| and n = r/r is the unit vector in the direction of observation, p (m) is the electric (magnetic) dipole moment, Q^e (Q^m) is the electric (magnetic) quadrupole tensor, and T is the tensor of the toroidal dipole moment [59].

The multipole decompositions are accomplished in both the Cartesian basis (source-representation) and the spherical basis (field-representation). The irreducible Cartesian mutipole moments are evaluated by [58].

$\begin{array}{ll}\text{p}=-\frac{1}{i\omega }\left\{\int d^{3}r{J}_{\alpha }^{\omega }{j}_0(kr)+\frac{k^2}{2}\int d^{3}r\left[3(r·{\text{J}}_{\omega })r_{\alpha }-r2J_{\alpha }^{\omega }\right]\frac{j_2(kr)}{{(kr)}^2}\right\}& (2)\end{array}$

$\begin{array}{ll}\text{m}=\frac{3}{2}{\int d^{3}r\left[\text{r}\times {\text{J}}_{\omega }\right]}_{\alpha }\frac{j_1(kr)}{kr}& (3)\end{array}$

$\begin{array}{l}{\text{Q}}^{\text{e}}=-\frac{3}{i\omega }\{{\displaystyle \int d^{3}r[3(r_{\alpha }{J}_{\beta }^{\omega }+J_{\alpha }^{\omega }{r}_{\beta })-2{\delta }_{\alpha \beta }(\text{r}·{\text{J}}_{\omega })]}\frac{j_1(kr)}{kr}\\ +2k^2{\displaystyle \int d^{3}r[5r_{\alpha }{r}_{\beta }(\text{r}·{\text{J}}_{\omega })-(r_{\alpha }{J}_{\beta }+J_{\alpha }{r}_{\beta })-r^2{\delta }_{\alpha \beta }(\text{r}·{\text{J}}_{\omega })]\frac{j_3(kr)}{{(kr)}^3}}\}& (4)\end{array}$

$\begin{array}{ll}{\text{Q}}^{\text{m}}=15{\displaystyle \int d^{3}r\{r_{\alpha }{[\text{r}\times {\text{J}}_{\omega }]}_{\beta }+r_{\beta }{[\text{r}\times {\text{J}}_{\omega }]}_{\alpha }\}\frac{j_2(kr)}{{(kr)}^2}}& (5)\end{array}$

where α, β = x, y, z, the electric current density is obtained by using J_ω (r) = -iωε₀(ε_r - ε_d) E_ω(r), where ε₀ = 8.845·10⁻¹² F/m is the permittivity of free space, ε_r is the relative permittivity of particle, E_ω (r) is electric field distribution. Multipole contributions show that the resonance peaks correspond to the overlap of several different multipole decomposition of the scattered field [59].

The scattering cross sections C_sca are defined from far-field scattered power (I) by normalizing to the energy flux of the incident wave (I_inc). The total scattering power can be obtained by summing the energy fluxes of multipoles which are integrations of the Poynting vector over the total solid angle,

$\begin{array}{ll}I=\frac{1}{8\pi {\epsilon }_0}[\frac{2{\omega }^4}{3c^3}{\left|\text{p}\right|}^2+\frac{2{\omega }^4}{3c^3}{\left|\text{m}\right|}^2+\frac{{\omega }^6}{20c^5}{\left|{\text{Q}}^{\text{e}}\right|}^2+\frac{{\omega }^6}{20c^5}{\left|{\text{Q}}^{\text{m}}\right|}^2]& (6)\end{array}$

$\begin{array}{ll}{C}_{\text{sca}}=\frac{I}{I_{\text{inc}}}& (7)\end{array}$

Here, ω is the angular frequency, c is the speed of light in a vacuum, the more high-order multipoles are not shown [59].

Figure 1A shows schematic of the multi-layered metal-dielectric-metal (MDM) nanoantenna. The nanoantenna is comprised of three identical gold strips, and two dielectric strips sandwiched by gold strips. Each strip has the same lengths l = 100 nm, different thicknesses (i.e., a thickness of gold strip d = 20nm and a thickness of dielectric strip t = 15 nm). The refractive index of the passive and active dielectric strip is n + iκ and n − iκ, respectively. Here the real parts of the refractive index are fixed as n = 1.44 while the non-Hermiticity parameter κ in imaginary parts is varied for different simulations. Note that regardless of the value of κ, loss and gain are always balanced in the system. The permittivity of gold is taken from Johnson and Christy [60]. For simplicity, the whole structure is assumed to be freestanding in air (ε₀ = 1) [61].

FIGURE 1

Figure 1. Optical response of the plasmonic antenna. (A) Schematic of the five layered plasmonic nanoantenna, composed of planar metallic strips separated by loss (n + iκ) and gain (n − iκ) materials. (B) Extinction cross section as a function of κ and the wavelengthλ. (C) Extinction (blue curves), scattering (red curves), and absorption (black curves) cross-sections for the same antenna of panel by calculated for three different κ: κ = 0 (top), κ = 0.25 (middle), and κ = 0.4 (bottom).

Results and Discussion

Figure 1B shows the extinction cross-section of the antenna, as a function of κ and λ. The incident plane wave, polarized in the y axis, is propagating along the x axis (see Figure 1A). All numerical calculations are performed with the finite element method (FEM) by COMSOL Multiphysics [62]. For a passive structure (i.e., κ = 0), the extinction cross-section shows two peaks corresponding to the excitations of plasmon ED and MD at shorter and longer wavelength, respectively [61]. With the increase of κ, the gain starts to compensate the loss of the system. One interesting feature is that the ED peak remains at the same wavelength of about 623 nm. Moreover, at a certain critical value (κ = 0.25 for this system), a region with negative extinction cross-section appears (see green area in Figure 1B). Beyond this critical point, the MD peak disappears and the extinction cross-section at the longer wavelength vanishes. The above behaviors are explored and demonstrated in details in Figure 1C, where the extinction (blue curves), scattering (red curves), and absorption (black curves) cross sections of the structure are plotted for three different values of κ. As anticipated, when κ = 0 (top panel), we observe two resonances that correspond to the ED and MD modes, respectively. Close to the critical point, κ = 0.25 (middle panel), the absorption cross-section (ACS) and extinction cross-section (ECS) becomes negative and predominant at the longer wavelength. With the amount of loss and gain increasing in the system, we observe the splitting of the MD. It suggests that one of the eigenmodes that is dark and not excited in the case of the passive system becomes bright when bringing loss and gain in the system. As κ is increased to 0.4 (bottom panel), the gain partially mitigates absorption losses, thus yielding a zero extinction at MD resonance. From the evolution of the MD and ED spectra based upon different κ in Figure 2, we can see that the MD mode shows strong dependence on κ, whereas the ED mode is almost unchanged. The sharp changes, occurring in the optical response of the antenna as κ approaches to the critical point, are a typical signature of a PT-symmetric system [42]. Therefore, associated with that behavior, we expect the system to exhibit an anisotropic response [3].

FIGURE 2

Figure 2. Evolution of the multiple moments spectra for different κ of the antenna with (A) κ = 0, (B) κ = 0.25, and (C) κ = 0.4.

To clarify the contributions of different modes, multipole decomposition including the electric dipole moment P, magnetic dipole moment M, electric quadrupole (EQ) moment Q^e, and magnetic quadrupole (MQ) moment Q^m can be obtained according to Khandekar et al. [57]. The radiated power of all the multipole moments sums over their contributions as:

$\begin{array}{ll}\text{I}=\frac{1}{8\pi {\epsilon }_0}[\frac{2{\omega }^4}{3{\text{c}}^3}{\left|\text{P}\right|}^2+\frac{2{\omega }^4}{3{\text{c}}^3}{\left|\text{M}\right|}^2+\frac{{\omega }^6}{20{\text{c}}^5}{\left|{\text{Q}}^{\text{e}}\right|}^2+\frac{{\omega }^6}{20{\text{c}}^5}{\left|{\text{Q}}^{\text{m}}\right|}^2]& (8)\end{array}$

In Figure 2, we show the multiple scattering spectra for κ = 0, κ = 0.25, and κ = 0.4. It is seen that the contributions from the induced ED and MD are significantly larger than those of EQ and MQ. Therefore, it is reasonable to neglect the high order multipole moments (EQ and MQ) that have negligible effects on the SCS for the three cases [61]. Clearly, it is seen that when κ = 0.4 the radiation from MD vanishes. Moreover, the green solid line in Figure 2 is the summation of the SCSs of the ED, MD, EQ, and MQ, which shows good agreement with the total SCS (black solid lines) obtained from the FEM simulation for the three cases, further confirming negligible contributions from other higher order modes [63].

To gain clearly understanding of the resonant dipole modes, we plot the surface charge distributions for two wavelength peak position of the SCS spectra when κ = 0 in Figure 3. Our previous work has shown that the first peak (i.e., λ = 610 nm) in this system corresponds to an electric dipole resonance in which the induced currents on the three plasmonic strips oscillate in phase [61], and the corresponding surface charge distribution is plotted in Figure 3A. The ED is induced by the metallic strips and it remains almost unchanged when varying κ, this can be confirmed in Figure 2 [58]. In order to better understand how the MD mode can be excited, the charge distribution of the other mode at λ = 778 nm is shown in Figure 3B, we can see that the forming strong circulating displacement currents in the both left two and right two metallicstrips induced the strong cavity magnetic dipole resonance mode. This kind of cavity mode is strongly affected by the material of dielectric layers (see Figure 2) [61]. Furthermore, as shown in Figures 2A,B, we can see that the ED and MD modes spectrally overlap in the spectrum and may have different radiation interferences that can shape the scattering pattern. The differential directionality (measured in decibels) of an antenna reads as follows [61, 63]:

$\begin{array}{l}D\text{(}\theta \text{,}\phi )=10\times {\text{log}}_{\text{10}}[4\pi S(\theta ,\phi )/{\displaystyle {\int }_{\phi }{\displaystyle {\int }_{\theta }S(\theta ,\phi )}}\sin (\theta )d\theta d\phi ],\\ 0\le \theta \le \pi ,0\le \phi \le 2\pi & (9)\end{array}$

Where θ and φ are spherical angles, and S(θ, φ) is the radiated power in the given direction θ and φ. Here, we are primarily interested in the forward-backward (FB) ratio G = D_F-D_B = 10 × log 10(S_F/S_B), where S_F and S_B are the far-field radiated powers in the forward and backward directions, respectively. The forward-backward ratio G allows a rough assessment of the directionality of the antennas [61]. The FB ratio G is plotted in Figure 4 as a function of wavelength λ and non-Hermiticity parameter κ. For a passive structure (i.e., κ = 0), we can see that G reaches about −30 dB at λ = 747 nm and nearly 34 dB at λ = 813 nm. Notice that positive(negative) G means that forward(backward) scattering dominates [61]. As κ increases, the gain starts to compensate the loss of the system, while both the peak and dip of Gare red-shifted and become broader. Interestingly, in the wavelength range from 807 to 885 nm, we can change the sign of Gat the same wavelength by tuning κ. Here we give two cases for λ = 835 nm and λ = 870 nm in Figures 4B,C, respectively. It is seen that for λ = 835 nm, G reaches the peak (dip) of +41 dB (−47 dB) when κ = 0.14 (κ = 0.34). Similarity, it is seen that for λ = 870 nm, G reaches the peak (dip) of +49 dB (−51 dB) when κ = 0.21 (κ = 0.3).

FIGURE 3

Figure 3. Surface charge distributions for the two resonant peaks [610 nm (A) and 778 nm (B)] when κ = 0 in Figure 2A.

FIGURE 4

Figure 4. Unidrectional scattering produced by the PT-symmeric structures. (A) The forward to backward ratio G as a function of κ and the wavelength. (B) G as a function of κ at λ = 835nm. (C) G as a function of κ at λ = 870nm.

The scattered electric farfield resulting from the combination of such p and m are as follows:

$\begin{array}{ll}\text{E}(\text{r})=\frac{k^2{\text{e}}^{ik·r}}{4\pi {\epsilon }_{0}r}\left[\text{n}\times (\text{p }\times \text{ n})+(\text{m }\times \text{ n})\text{+}\dots \right]& (10)\end{array}$

Where p(m) is the dipole moment of the ED (MD), kis the wave vector, n = k/|k|is the unit vector in the emission direction, and r is the coordinate vector. According to Equation (10), zero forward or backward scattering requires (1) the two dipoles (ED and MD) are orthogonal to each other, (2) their radiated powers are nearly identical, and (3) the phase difference Δφ = φ_p − φ_m = 0 (forward scattering) or Δφ = ±π (backward scattering), where φ_p and φ_m are the relative phase of the induced p and m in the nanoantenna. In our case, when Δφ = φ_p−φ_m = 0 is fulfilled (i.e., the first Kerker condition) [64], most radiated power is directed to the left half space (+xdirection). Likewise, when Δφ = φ_p−φ_m = ±π (i.e., the second Kerker condition) is nearly fulfilled, scattering to the right half space (−xdirection) dominates [61]. In our system, it is reasonable to assume the ED and MD to be oriented along the corresponding vectors of the incident field. It means that the induced electric and magnetic dipole moments of the antenna in Figure 1A should be p = (0, p_y, 0) and m = (0, 0, m_z), respectively. To demonstrate the first and second Kerker conditions can be switched at the same wavelength by adjusting κ, we take the case shown in Figure 4C (i.e., λ = 870 nm) as the example. Figure 5 shows the normalized radiated powers (left axis) and the phase difference (right axis) of the induced dipole moments p_y and m_z as a function of the non-Hermiticity parameter κ. It is seen that at κ = 0.21 the radiated powers of p_y and m_z have comparable amplitudes (see the dashed curve in Figure 5) and relatively small phase difference Δφ = 0.09π (see the green solid curve in Figure 5), thus the first Kerker condition is approximately reached. In a similar way, the second Kerker condition is nearly met at κ = 0.3 with Δφ = 0.94π. We note that the first (second) Kerker condition can be achieved at all the peaks (dips) of G which corresponding to the red (blue) area in Figure 4A (results not shown here).

FIGURE 5

Figure 5. The normalized radiated powers of ED and MD moment and their relative phase difference Δφ for λ = 870nm.

In Figures 6A,B, we plot the 2D far-field scattering patterns in xoz plane at λ = 835 nm for κ = 0.14 and κ = 0.34, respectively. It shows that an almost complete cancellation of the radiation toward the left-half space (+x direction) and a predominated radiation toward to the right-half space (−x direction) for κ = 0.14 (see Figure 6A). In sharp contrast, for κ = 0.34, the radiated power scatters almost completely toward the −x direction (see Figure 6B) [61]. Similar features can be seen for κ = 0.21 and κ = 0.3 when λ = 870 nm as shown in Figures 6C,D. To better characterize the directivity of the scattering, we also label the main lobe angular beam-width α which corresponds to the angle for the full width at half-maximum of the differential scattering intensity [63], as shown in Figure 6. It is seen that for λ = 835 nm α is 62° when κ = 0.14 and 63° when κ = 0.34. For λ = 870 nm shown in Figures 6C,D, α is 88° when κ = 0.21 and 91° when κ = 0.3. Figure 6 further shows that the scattering direction of the antenna at a fixed wavelength can be reversed by adjusting κ.

FIGURE 6

Figure 6. 2D radiation patterns in the xoz plane. (A,B) Scattering pattern with κ = 0.14 and κ = 0.34 at λ = 835nm, respectively. (C,D) Scattering pattern with κ = 0.21 and κ = 0.3 at λ = 870nm, respectively.

In order to explore more scattering properties of the PT-symmetric systems, we investigated a series of five-layer plasmonic nanoantennas. First, a five-layer plasmonic nanoantenna, composed of planar metallic strips separated by two materials with different amount of gains, n-iκ₁ and n-iκ₂, is simulated as shown in Supplementary Figure 1. There is no positive and negative change of unidirectivity in this system. The unidirectivity keeps positive at all values of κ₁ and κ₂. Secondly, a five-layer plasmonic nanoantenna, composed of planar metallic strips separated by two materials with different amount of losses, n+iκ₁ and n+iκ₂, is simulated as shown in Supplementary Figure 2. Similarly, there is no positive and negative change of unidirectivity and the unidirectivity keeps positive at all values of κ₁ and κ₂. Finally, the previous constructed PT-symmetric structure is also calculated with different loss (n+iκ₁) and gain (n–iκ₂) materials, as shown in Supplementary Figure 3. In the results, it is shown that the unidirectivity could switch between positive and negative with the change of κ₁ and κ₂. When κ₁ = κ₂ = κ, the results are coincident with the previous results in Figure 4. In order to investigate the presence of critical point, we describe state coalescence and power flow along the waveguide, as shown in Supplementary Figure 4.

We also studied the opposite incidence (-x direction, from right to left) in the PT-symmetric system, as shown in Supplementary Figure 5. The forward-backward ratio G results are smaller than the positive incidence results in Figure 4. The transmission and reflection properties of the PT-symmetric structure are simulated in plane wave incidence at λ = 835 nm and λ = 870 nm (see Supplementary Figure 6). The peaks(dips) of transmissivity/reflectivity ratio basically correspond to the peaks(dips) of G in Figure 4C. It is demonstrated that the positive and negative unidirectivities are related to transmission and reflection enhancements.

In Figures 7B,C, we show the scattering patterns in xoz plane by putting the antennas in a chain along y axis. The operating wavelength is λ = 870 nm and the inter-particle distance is fixed at d₀ = 300 nm. Significant reduction in α is obtained with increasing number of antennas N due to the constructive far-field interferences, which is quite similar to previously reported study in high-index dielectric particle chain of longitudinal configuration [63]. The operating wavelength of λ = 870 nm can offer the best directionality with the narrowest α of 5.6° for κ = 0.21 and 5.8° for κ = 0.3 when N = 6 [63]. As a result, arranging the antennas into an array can achieve needle-like radiation [65].

FIGURE 7

Figure 7. (A) Chain of the PT-symmetric structure with inter-particle distance d. (B,C) Scattering patterns in xoz plane by a chain such particles with N = 1, 2, 4, and 6 for κ = 0.21 and κ = 0.3 at λ = 870nm, respectively.

Considering low values of non-Hermiticity parameter, we also redesigned a five-layer plasmonic nanoantenna with the geometric parameters (l₁ = 30 nm, d₁ = 8 nm, t₁ = 6 nm), as shown in Supplementary Figure 7. For an available gain material with the κ ≤ 0.2, the tunable unidirectivity could also be realized in designed structure. In addition, the structure parameters could be further optimized to obtain excellent performance, and we will research more about it in the following work.

Conclusions

In conclusion, we have studied the scattering properties of a multi-layered MDM plasmonic nanoantena with balanced gain and loss in the dielectric layers. We showed that the non-Hermiticity parameter has strong influences on the total cross sections and the scattering directionality of the antenna. In particular, the antenna exhibits unidirectional scattering which can be tuned by changing the non-Hermiticity parameter κ. These interesting scattering features of the antenna can be understood by the phase shifts between the electric and magnetic dipole moments induced in the asymmetric material composition. Our results are useful in designing unidirectional plasmonic nanoantennas with active materials.

Data Availability Statement

All datasets generated for this study are included in the manuscript/Supplementary Files.

Author Contributions

HL and XZ conceived the idea and supervised the whole study. XZ, CX, and KC conducted the numerical calculations and drafted the first manuscript. XZ, CX, XS, QL, KC, CW, ZW, and HL derived the theory and carried out the analysis. All authors contributed to the review of manuscript.

Conflict of Interest

The authors declare that the research was conducted in the absence of any commercial or financial relationships that could be construed as a potential conflict of interest.

Acknowledgments

This work was supported by National Natural Science Foundation of China (NSFC) (11174221, 11204218, 11404213, 11674248, 61205041, 11174057); supported by the Fundamental Research Funds for the Central Universities.

Supplementary Material

The Supplementary Material for this article can be found online at: https://www.frontiersin.org/articles/10.3389/fphy.2019.00161/full#supplementary-material

References

1. Zhang X, Xiao J, Zhang Q, Li L, Yao Y. Plasmonic TM-like cavity modes and the hybridization in multilayer metal-dielectric nanoantenna. Opt Exp. (2015) 23:16122–32. doi: 10.1364/OE.23.016122

PubMed Abstract | CrossRef Full Text | Google Scholar

2. Halas NJ, Lal S, Chang W, Link S, Nordlander P. Plasmons in strongly coupled metallic nanostructures. Chem Rev. (2011) 111:3913–61. doi: 10.1021/cr200061k

PubMed Abstract | CrossRef Full Text | Google Scholar

3. Manjavacas A. Anisotropic optical response of nanostructures with balanced gain and loss. ACS Photon. (2016) 3:1301–7. doi: 10.1021/acsphotonics.6b00274

CrossRef Full Text | Google Scholar

4. O'Neal DP, Hirsch LR, Halas NJ, Payne JD, West JL. Photo-thermal tumor ablation in mice using near infrared absorbing nanoparticles. Cancer Lett. (2004) 209:171–6. doi: 10.1016/j.canlet.2004.02.004

PubMed Abstract | CrossRef Full Text | Google Scholar

5. Alvarez-Puebla R, Liz-Marzán LM, Abajo FJGD. Light concentration at the nanometer scale. J Phys Chem Lett. (2010) 1:2428–2434. doi: 10.1021/jz100820m

CrossRef Full Text | Google Scholar

6. Atwater HA, Polman A. Plasmonics for improved photovoltaic devices. Nat Mater. (2010) 9:205–13. doi: 10.1038/nmat2629

PubMed Abstract | CrossRef Full Text | Google Scholar

7. Khurgin JB. How to deal with the loss in plasmonics and metamaterials. Nat Nanotechnol. (2015) 10:2–6. doi: 10.1038/nnano.2014.310

PubMed Abstract | CrossRef Full Text | Google Scholar

8. Nezhad M, Tetz K, Fainman Y. Gain assisted propagation of surface plasmon polaritons on planar metallic waveguides. Opt Exp. (2004) 12:4072–9. doi: 10.1364/OPEX.12.004072

PubMed Abstract | CrossRef Full Text | Google Scholar

9. Gather MC, Meerholz K, Danz N, Leosson K. Net optical gain in a plasmonic waveguide embedded in a fluorescent polymer. Nat Photonics. (2010) 7:457–61. doi: 10.1038/nphoton.2010.121

CrossRef Full Text | Google Scholar

10. Hess O, Pendry JB, Maier SA, Oulton RF, Hamm JM, Tsakmakidis KL. Active nanoplasmonic metamaterials. Nat Mater. (2012) 11:573–84. doi: 10.1038/nmat3356

PubMed Abstract | CrossRef Full Text | Google Scholar

11. Zhang X, Xiao J, Zhang Q. Interaction between single nano-emitter and plasmonic disk–ring nanostructure with multiple Fano resonances. J Opt Soc Am B. (2014) 31:2193–200. doi: 10.1364/JOSAB.31.002193

CrossRef Full Text | Google Scholar

12. Noginov MA, Podolskiy VA, Zhu G, Mayy M, Bahoura M, Adegoke JA, et al. Compensation of loss in propagating surface plasmon polariton by gain in adjacent dielectric medium. Opt Exp. (2008) 16:1385–92. doi: 10.1364/OE.16.001385

PubMed Abstract | CrossRef Full Text | Google Scholar

13. Xian J, Chen L, Niu H, Qu J, Song J. Significant field enhancements in an individual silver nanoparticle near a substrate covered with a thin gain film. Nanoscale. (2004) 6:13994–4001. doi: 10.1039/C4NR03678F

PubMed Abstract | CrossRef Full Text | Google Scholar

14. Song J, Xian J, Yu M, Wang D, Ye S, Niu H, et al. Ultrahigh enhancement factor by using a silver nanoshell with a gain core above a silver substrate for surface-enhanced Raman scattering at the single-molecule level. IEEE Photon J. (2015) 7:1–8. doi: 10.1109/JPHOT.2015.2481599

CrossRef Full Text | Google Scholar

15. Stockman MI. Spaser action, loss compensation, and stability in plasmonic systems with gain. Phys Rev Lett. (2011)106:156802. doi: 10.1103/PhysRevLett.106.156802

PubMed Abstract | CrossRef Full Text | Google Scholar

16. Lozano G, Louwers DJ, Rodriguez SRK, Murai S, Jansen OTA, Verschuuren MA, et al. Plasmonics for solid state lighting:enhanced excitation and directional emission of highly efficient light sources. Light. (2013) 2:e66. doi: 10.1038/lsa.2013.22

CrossRef Full Text | Google Scholar

17. Liu K, Li N, Sadana DK, Sorger VJ. Integrated nanocavity plasmon light sources for on-chip optical interconnects. ACS Photonics. (2016) 3:233–42. doi: 10.1021/acsphotonics.5b00476

CrossRef Full Text | Google Scholar

18. Bergman DJ, Stockman MI. Surface plasmon amplification by stimulated emission of radiation: quantum generation of coherent surface plasmons in nanosystems. Phys Rev Lett. (2003) 90:027402. doi: 10.1103/PhysRevLett.90.027402

PubMed Abstract | CrossRef Full Text | Google Scholar

19. Stockman MI. Spasers explained. Nat Photonics. (2008) 2:327–9. doi: 10.1038/nphoton.2008.85

CrossRef Full Text | Google Scholar

20. Zheludev NI, Prosvirnin SL, Papasimakis N, Fedotov VA. Lasing spaser. Nat Photonics. (2008) 2:351–4. doi: 10.1038/nphoton.2008.82

CrossRef Full Text | Google Scholar

21. Noginov MA, Zhu G, Belgrave AM, Bakker R, Shalaev VM, Narimanov EE, et al. Demonstration of a spaser-based nanolaser. Nature. (2009) 460:1110–2. doi: 10.1038/nature08318

PubMed Abstract | CrossRef Full Text | Google Scholar

22. Oulton RF, Sorger VJ, Zentgraf T, Ma RM, Gladden C, Dai L, et al. Plasmon lasers at deep subwavelength scale. Nature. (2009) 461:629–32. doi: 10.1038/nature08364

PubMed Abstract | CrossRef Full Text | Google Scholar

23. Sorger VJ, Zhang X. Spotlight on plasmon lasers. Science. (2011) 333:709–10. doi: 10.1126/science.1204862

PubMed Abstract | CrossRef Full Text | Google Scholar

24. Berini P, Leon ID. Surface plasmon-polariton amplifiers and lasers. Nat Photonics. (2012) 6:16–24. doi: 10.1038/nphoton.2011.285

CrossRef Full Text | Google Scholar

25. Zhou W, Dridi M, Suh JY, Kim CH, Co DT, Wasielewski MR, et al. Lasing action in strongly coupled plasmonic nanocavity arrays. Nat Nanotechnol. (2013) 8:506–11. doi: 10.1038/nnano.2013.99

PubMed Abstract | CrossRef Full Text | Google Scholar

26. Yang A, Odom TW. Breakthroughs in photonics 2014: advances in plasmonic nanolasers. IEEE Photonics J. (2015) 7:1–6. doi: 10.1109/JPHOT.2015.2413773

CrossRef Full Text | Google Scholar

27. Ho J, Tatebayashi J, Sergent S, Fong CF, Iwamoto S, Arakawa Y. Low-threshold near-infrared GaAs-AlGaAs core-shell nanowire plasmon laser. ACS Photonics. (2015) 2:165–71. doi: 10.1021/ph5003945

CrossRef Full Text | Google Scholar

28. Krasavin AV, Vo TP, Dickson W, Bolger PM, Zayats AV. All-plasmonic modulation via stimulated emission of copropagating surface plasmon polaritons on a substrate with gain. Nano Lett. (2011) 11:2231–35. doi: 10.1021/nl200255t

PubMed Abstract | CrossRef Full Text | Google Scholar

29. Zhu W, Premaratne M, Gunapala SD, Agrawal GP, Stockman MI. Quasi-static analysis of controllable optical crosssections of a layered nanoparticle with a sandwiched gain layer. J Opt. (2014) 16:075003. doi: 10.1088/2040-8978/16/7/075003

CrossRef Full Text | Google Scholar

30. Bender CM, Boettcher S. Real spectra in non-hermitian hamiltonians having PT symmetry. Phys Rev Lett. (1998) 80:5243–6. doi: 10.1103/PhysRevLett.80.5243

CrossRef Full Text | Google Scholar

31. El-Ganainy R, Makris KG, Christodoulides DN, Musslimani ZH. Theory of coupled optical PT-symmetric structures. Opt Lett. (2007) 32:2632–4. doi: 10.1364/OL.32.002632

PubMed Abstract | CrossRef Full Text | Google Scholar

32. Klaiman S, Günther U, Moiseyev N. Visualization of branch points in PT-symmetric waveguides. Phys Rev Lett. (2008) 101:080402. doi: 10.1103/PhysRevLett.101.080402

PubMed Abstract | CrossRef Full Text | Google Scholar

33. Longhi S. Bloch oscillations in complex crystals with PT symmetry. Phys Rev Lett. (2009) 103:123601. doi: 10.1103/PhysRevLett.103.123601

PubMed Abstract | CrossRef Full Text | Google Scholar

34. Ruter CE, Makris KG, El-Ganainy R, Christodoulides DN, Segev M, Kip D. Observation of parity-time symmetry in optics. Nat Phys. (2010) 6:192–5. doi: 10.1038/nphys1515

CrossRef Full Text | Google Scholar

35. Kulishov M, Laniel JM, Bélanger N, Azaña N, Plant DV. Nonreciprocal waveguide Bragg gratings. Opt Exp. (2005) 13:3068–78. doi: 10.1364/OPEX.13.003068

PubMed Abstract | CrossRef Full Text | Google Scholar

36. Miri MA, Eftekhar MA, Facao M, Abouraddy AF, Bakry A, Razvi MAN, et al. Scattering properties of PT-symmetric objects. J Opt. (2016) 18:075104. doi: 10.1088/2040-8978/18/7/075104

CrossRef Full Text | Google Scholar

37. Lin Z, Ramezani H, Eichelkraut T, Kottos T, Cao H, Christodoulides DN. Unidirectional invisibility induced by PT symmetric periodic structures. Phys Rev Lett. (2011) 106:213901. doi: 10.1103/PhysRevLett.106.213901

PubMed Abstract | CrossRef Full Text | Google Scholar

38. Longhi S. Invisibility in PT-symmetric complex crystals. J Phys A. (2011) 44:2813–21. doi: 10.1088/1751-8113/44/48/485302

CrossRef Full Text | Google Scholar

39. Lupu A, Benisty H, Degiron A. Using optical PT-symmetry for switching applications. Phot Nano Fundam Appl. (2014) 12:305–11. doi: 10.1016/j.photonics.2014.05.003

CrossRef Full Text | Google Scholar

40. Rivolta NXA, Maes B. Diffractive switching by interference in a tailored PT-symmetric grating. J Opt Soc Am. (2015) 32:1330–7. doi: 10.1364/JOSAB.32.001330

CrossRef Full Text | Google Scholar

41. Miroshsnichenko AE, Malomed BA, Kivshar YS. Nonlinearly PT-symmetric systems: spontaneous symmetry breaking and transmission resonances. Phys Rev. (2011) 84:911–6. doi: 10.1103/PhysRevA.84.012123

CrossRef Full Text | Google Scholar

42. Guo A, Salamo GJ, Duchesne D, Morandotti R, Volatier-Ravat M, Aimez V, et al. Observation of PT-symmetry breaking in complex optical potentials. Phys Rev Lett. (2009) 103:093902. doi: 10.1103/PhysRevLett.103.093902

PubMed Abstract | CrossRef Full Text | Google Scholar

43. Jia Y, Yan Y, Kesava SV, Gomez ED, Giebink NC. Passive parity-time symmetry in organic thin film waveguides. ACS Photonics. (2015) 2:319–25. doi: 10.1021/ph500459j

CrossRef Full Text | Google Scholar

44. Peng B, Özdemir SK, Lei F, Monifi F, Gianfreda M, Long GL, et al. Parity-timesymmetric whispering-gallery microcavities. Nat Phys. (2014) 10:394–8. doi: 10.1038/nphys2927

CrossRef Full Text | Google Scholar

45. Regensburger A, Bersch C, Miri MA, Onishchukov G, Christodoulides DN, Peschel U. Parity-time synthetic photonic lattices. Nature. (2012) 488:167–71. doi: 10.1038/nature11298

PubMed Abstract | CrossRef Full Text | Google Scholar

46. Wimmer M, Regensburger A, Miri MA, Bersch C, Christodoulides DN, Peschel U. Observation of optical solitons in PT-symmetric lattices. Nat Commun. (2015) 6:394–8. doi: 10.1038/ncomms8782

PubMed Abstract | CrossRef Full Text | Google Scholar

47. Benisty H, Degiron A, Lupu A, Lustrac AD, Chénais S, Forget S, et al. Implementation of PT symmetric devices using plasmonics:principle and applications. Opt Exp. (2011) 19:18004–19. doi: 10.1364/OE.19.018004

PubMed Abstract | CrossRef Full Text | Google Scholar

48. Alaeian H, Dionne JA. Non-hermitian nanophotonic and plasmonic waveguides. Phys Rev B. (2014) 89:188–92. doi: 10.1103/PhysRevB.89.075136

CrossRef Full Text | Google Scholar

49. Alaeian H, Dionne JA. Parity-time-symmetric plasmonic metamaterials. Phys Rev A. (2014) 89:429–35. doi: 10.1103/PhysRevA.89.033829

CrossRef Full Text | Google Scholar

50. Alaeian H, Dionne JA. Controlling electric, magnetic, and chiral dipolar emission with PT-symmetric potentials. Phys Rev B. (2015) 91:245108. doi: 10.1103/PhysRevB.91.245108

CrossRef Full Text | Google Scholar

51. Baum B, Alaeian H, Dionne JA. A parity-time symmetric coherent plasmonic absorber-amplifier. J Appl Phys. (2015) 117:063106. doi: 10.1063/1.4907871

CrossRef Full Text | Google Scholar

52. Mattheakis M, Oikonomou T, Molina MI, Tsironis GP. Phase transition in PT symmetric active plasmonic systems. IEEE J Sel Top Quant Electron. (2016) 22:76–81. doi: 10.1109/JSTQE.2015.2490018

CrossRef Full Text | Google Scholar

53. Sounas DL, Fleury R, Alù A. Unidirectional cloaking based on metasurfaces with balanced loss and gain. Phys Rev Appl. (2015) 4:014005. doi: 10.1103/PhysRevApplied.4.014005

CrossRef Full Text | Google Scholar

54. Lupu A, Benisty H, Degiron A. Switching using PT symmetry in plasmonic systems: positive role of the losses. Opt Exp. (2013) 21:21651–68. doi: 10.1364/OE.21.021651

PubMed Abstract | CrossRef Full Text | Google Scholar

55. Alaeian H, Baum B, Jankovic V, Lawrence M, Dionne JA. Towards nanoscale multiplexing with parity-time symmetric plasmonic coaxial waveguides. Phys Rev B. (2016) 93:205439. doi: 10.1103/PhysRevB.93.205439

CrossRef Full Text | Google Scholar

56. Jin W, Khandekar C, Pick A, Polimeridis AG, Rodriguez AW. Amplified and directional spontaneous emission from arbitrary composite bodies: a self-consistent treatment of Purcell effect below threshold. Phys Rev B. (2016) 93:433–46. doi: 10.1103/PhysRevB.93.125415

CrossRef Full Text | Google Scholar

57. Khandekar C, Jin W, Miller OD, Pick A, Rodriguez AW. Giant frequency-selective near-field energy transfer in active-passive structures. Phys Rev B. (2016) 94:115402. doi: 10.1103/PhysRevB.94.115402

CrossRef Full Text | Google Scholar

58. Alaee R, Rockstuhl C, Fernandez-Corbaton I. An electromagnetic multipole expansion beyond the long-wavelength approximation. Opt Commun. (2018) 407:17–21. doi: 10.1016/j.optcom.2017.08.064

CrossRef Full Text | Google Scholar

59. Xu C, Cheng K, Li Q, Shang X, Wu C, Wei Z, et al. The dual-frequency zero-backward scattering realized in a hybrid metallo-dielectric nanoantenna. AIP Adv. (2019) 9:075121. doi: 10.1063/1.5099533

CrossRef Full Text | Google Scholar

60. Johnson PB, Christy RW. Optical constants of the noble metals. Phys Rev B. (1972) 6:4370–9. doi: 10.1103/PhysRevB.6.4370

CrossRef Full Text | Google Scholar

61. Zhang X, Xiao J, Zhang Q, Qin F, Cai X, Ye F. Dual-band unidirectional emission in a multilayered metal–dielectric nanoantenna. ACS Omega. (2017) 2:774–83. doi: 10.1021/acsomega.7b00121

PubMed Abstract | CrossRef Full Text | Google Scholar

62. Available, online at: http://www.comsol.com (accessed July 01, 2019).

Google Scholar

63. Zhang X, Zhang Q, Zeng S, Liu Z, Xiao J. Dual-band unidirectional forward scattering with all-dielectric hollow nanodisk in the visible. Opt Lett. (2018) 43:1275–8. doi: 10.1364/OL.43.001275

PubMed Abstract | CrossRef Full Text | Google Scholar

64. Kerker M, Wang DS, Giles CL. Electromagnetic scattering by magnetic particles. J Opt Soc Am B. (1983) 73:765–7. doi: 10.1364/JOSA.73.000765

CrossRef Full Text | Google Scholar

65. Ziolkowski RW. Using Huygens multiple arrays to realize unidirectional need-like radiation. Phys Rev X. (2017) 7:031017. doi: 10.1103/PhysRevX.7.031017

CrossRef Full Text | Google Scholar