Original Article | Open Access | Published:

Chiral surface waves supported by biaxial hyperbolic metamaterials

Light: Science & Applications volume 4, page e328 (2015) | Download Citation

Subjects

Abstract

We discover a new kind of surface wave on biaxial hyperbolic metamaterial, which, in the k-space, connects the two diabolical points (or conical singularities) of the equifrequency surface. Interestingly, the propagation of such surface wave is found to be sensitive to the refractive index of the surrounding dielectric medium, showing a convex, concave or flat phase front when the refractive index is varied. Furthermore, the surface wave shows an elliptically polarized state, in which helicity is dependent on the propagation direction. This feature can be utilized for the spin-controllable excitation of surface waves, opening a gateway towards integrated photonic circuits with reconfigurable functionalities.

Introduction

The existence of electromagnetic (EM) waves on two-dimensional interfaces has been extensively studied over the last several decades. The most widely studied surface wave is surface plasmonic polariton (SPP)1,2,3,4, which normally exists at the interface between a noble metal and a dielectric. Because of the unique properties of strong field confinement and intensity enhancement, SPPs have been extensively explored in applications like super-resolution imaging5,6,7, bio-sensing8,9, wave guiding9,10,11 and photolithography12,13. Recently, it has been shown that by nanostructuring the metal surface, it is possible to modify the dispersion of SPPs or excite the SPPs in a prescribed manner14,15,16,17,18,19. It has also been shown that surface waves can exist at the interface between an anisotropic dielectric medium and isotropic dielectric medium when a certain relationship between the dielectric constants is satisfied. This type of surface wave, so-called Dyakonov waves20,21, are loss free, in sharp contrast to SPPs, which suffer from Ohmic loss. Dyakonov-wave-like surface waves are also supported on layered hyperbolic metamaterials and on photonic crystals with enhanced angle range under the long-wavelength limit22,23.

Hyperbolic metamaterials, a special kind of anisotropic metamaterial whose dielectric tensor elements have mixed signs, have attracted growing attention recently because they support very large wave vectors. Their exotic features enable many intriguing applications, such as sub-wavelength imaging24,25,26,27, hyper-lens28,29,30 and enhanced spontaneous and thermal emissions31,32,33 that are infeasible with natural materials. While most studies have focused on uniaxial hyperbolic metamaterials, it has been shown recently that by introducing in-plane anisotropy, the quadratic degeneracy point splits into two diabolical points in the equifrequency surface, and conical diffraction with different topological features from a conventional biaxial media has been investigated34. In this letter, we demonstrate the existence of a new kind of surface wave between a biaxial hyperbolic metamaterial (BHM) and an isotropic dielectric material. In contrast to extensively studied surface waves such as SPPs and Dyankonov waves, whose in-plane wave vector is greater than that of the bulk modes, the in-plane wave vector of the surface wave supported by BHM lies between two bulk modes. Interestingly, the wavefront of the surface mode can be convex, concave or flat, by varying the refractive index of the surrounding dielectric medium. More remarkably, in general, the surface wave shows an elliptically polarized state, in which helicity is dependent on the propagation direction, leading to spin-controlled excitation of the surface wave.

Materials and methods

Without loss of generality, BHM’s permittivity tensor can be written as diag[εx, εy, εz], with εz being negative and εx < εy being positive. Under Heaviside-Lorentz units, the general Fresnel equation for an equifrequency contour (EFC) can be expressed as A typical EFC of a lossless biaxial hyperbolic metamaterial is shown in Figure 1a. There exist four singular points in the kx-kz plane located at . These singular points are reminiscent of the Dirac points for electrons extensively investigated in graphene, but in the momentum space. Next, we numerically solve for surface waves at the interface between the BHM and an isotropic dielectric material, which involves searching for hybrid modes composed of both transverse-electric and transverse-magnetic (TE and TM) polarizations. The interface is in the x-z plane, where z represents the direction with negative permittivity and x is the direction with the smaller permittivity tensor. Similar to Dyakonov waves, the surface wave supported at the surface of the BHM involves both eigenmodes inside the metamaterial and TE and TM waves in the surrounding dielectric medium. For ease of discussion, we define a local coordinate frame [x′, y, z′] with z′ defined to be along the propagation direction of the surface wave (Figure 1c). In this local frame, the components of the TM and TE mode in the surrounding dielectric medium with relative permittivity εs can be expressed in the local frame as: where kTM and kTE are the decay constants along the y direction for the TM and TE mode, respectively, and q is the wave vector along the z′ direction. Components of the two eigenmodes inside the metamaterial can be numerically solved by substituting solutions of Equation (1) into Maxwell Equations. Finally, all the tangential E and H components of the four modes can be written into a characteristic matrix: Boundary conditions at the interface require that the tangential components of electric field and magnetic field are matched. In order to obtain the surface mode, we search through the kx and kz parameter space to find the existence of a nonzero solution by calculating the rank of the matrix . Specifically, the boundary condition at the corresponding point is perfectly matched when the rank of the matrix is reduced to 3.

Figure 1
Figure 1

(a) 3D equi-frequency surface of a biaxial hyperbolic material. (b) On the interface between biaxial hyperbolic material and normal covering medium, an anomalous surface wave exists in the gap between degeneracy points. (c) Configuration of a realistic structure to realize BHM. The Si/SiO2 multilayer dielectric structure provides large in-plane anisotropy, while the embedded metallic nanowires lead to a negative permittivity along the z direction. The unit cell of the BHM has dimensions px× py = 120 × 60 nm × nm, which is a deep subwavelength to minimize the nonlocality of the system. The ratio of the Si and SiO2 segments are all 0.5 in a unit cell. The diameter of the Ag nano-wires is 18 nm, which is less than the skin depth of silver.

The dispersion of the surface waves for different refractive indices of the surrounding medium is shown in Figure 1b. Here, we set εx = 4.6, εy = 8.6 and εz = –3.62, which are retrieved by using the generalized Maxwell-Garnett theory35 from a realistic composite structure given in Figure 1c. The structure consists of a Si/SiO2 multilayer medium (stacked along x direction) with an array of metallic nanowires oriented along the z direction embedded inside the layered medium. It was discovered that when the refractive index of the surrounding medium εs satisfies εx < εs < εy, a surface state exists whose equifrequency curve connects the two diabolical points. When εs is increased, the equifrequency curve gradually evolves from a concave shape to a convex one. At , the dispersion becomes flat, indicating that the surface wave can propagate without diffraction. An analytical solution of the effective index of the surface mode can be obtained for kx = 0, which gives the result: . Because the EFCs of the surface waves always connect the diabolic points, then by setting kz = kDz, the condition for generating a flat dispersion can be obtained.

Results and discussion

To verify the effective medium description for the nanowire medium, we numerically solve the dispersion of the surface mode by using COMSOL. Both the real and imaginary parts of the mode index are shown in Figure 2. The numerically calculated mode index for the nanowire medium matches reasonably well with that which is obtained analytically by the effective medium approach, with a transition of the phase-front from concave to convex when the refractive index of the surrounding medium decreases. The slight deviations from the ideal effective medium case may be caused by nonlocalities36. As realistic metal parameters are used, there is ohmic loss in the system, leading to an imaginary part of the mode index, as shown in Figure 2b. However, the nanowire medium exhibits significantly lower optical loss than the effective medium because the effective medium formulism assumes a homogeneous distribution of the electric field inside the nanowire. Interestingly, for both effective medium and nanowire structure, the surface mode with a smaller refractive index εs of the surrounding medium exhibits higher loss for both the effective medium and nanowire structure. This trend is due to the greater z component of the electric field inside the hyperbolic medium with smaller εs.

Figure 2
Figure 2

Real (a) and imaginary part (b) of mode indexes for different ns. Results for effective medium and real structures are shown in solid lines and circles, respectively.

To calculate the surface state in BHM, we carry out full-wave simulations at a wavelength of 1550 nm with both the homogenous effective medium (Figure 3a, 3b and 3c) and the realistic metamaterial structure (Figure 3d, 3e and 3f). In the effective medium simulation, no loss is included in the effective parameters. In the simulation, the surface waves are excited by a linearly polarized Gaussian wave incident along the y-direction at one side, with the centre of the Gaussian beam aligned with the interface. The y components of the electric fields for different refractive indices of the surrounding medium are shown in Figure 3, exhibiting flat, convex and concave wavefronts at ns = 2.3, 1.9 and 2.8, respectively (Figure 3a, 3b and 3c). The field pattern (Figure 3d, 3e and 3f) of the realistic metamaterial structure shows very similar features to that of the effective medium, in spite of the intensity attenuation along the propagation direction due to the Ohmic loss of the metal nanowires. The simulation results of the propagation of the surface wave in both the effective medium and realistic structures agree very well with the equifrequency curve shown in Figure 1b. Here, the diffractionless propagation of the surface wave is a close analogue to spatial solitons in nonlinear optics, but is purely based on linear properties of the biaxial metamaterial and the surrounding dielectric and therefore suitable for wave guiding at low optical intensities. In addition, the sensitivity of the wavefront to the refractive index of the surrounding medium may lead to the application of the BHM as a refractive index sensor. An estimation of the coupling efficiency is obtained by numerically integrating the power of surface waves. For the effective medium, the coupling efficiency for a y-polarized incident wave is 39.7%, 46.3% and 48.5% for ns =1.9, 2.3 and 2.8, respectively. The coupling efficiency for the nanowire medium is numerically calculated to be 32.5% at ns =1.9, which is slightly lower than that of the effective medium.

Figure 3
Figure 3

The flat, concave and convex wave-fronts of the surface wave supported by a biaxial hyperbolic metamaterial. (a, b, c) Simulation of the field distribution (Ey) of the surface wave at the interface between an isotropic dielectric medium and the biaxial hyperbolic effective medium. The refractive indices of surrounding medium for (a), (b) and (c) are nc = 2.3, 1.9 and 2.8, respectively. (d, e, f) The same as (a, b, c), but with the effective medium replaced by the realistic metamaterial structures.

The polarization state of the surface mode is obtained from the non-zero solution of the aforementioned characteristic matrix. From the field basis used in matrix , we can express the total transverse field components in x′ and y directions in the surrounding medium and BHM as [iγ, kz’] and [iγ, εykz’], respectively. Here, and is the ratio between the coefficients of TE and TM modes obtained from the nonzero solution of matrix . The plot of γ vs kx is shown in Figure 4a. For kx =0, the surface wave is purely TM-polarized; thus, the amplitude of TE is zero. Interestingly, the phase difference between the TE and TM components is constantly for positive kx and for negative kx. This means that the electric field in the surrounding medium is elliptically polarized, with both the sign and magnitude of the ellipticity dependent on kx, as shown in Figure 4b–4j. The polarization state of the surface wave inside the BHM preserves the same handedness as in the surrounding medium due to the boundary condition across the interface.

Figure 4
Figure 4

(a) The ratio of the amplitude of the TE to TM mode in surrounding medium. The phase difference between the two modes is ±π/2, leading to an elliptically polarized mode for nonzero kx. The red, blue and green curves correspond to ns =1.9 (concave), 2.3 (flat) and 2.8 (convex), respectively. (bj) Polarization in both surrounding medium (red) and BHM (blue) under different kx and ns. For positive (negative) kx, surface waves show right (left) handedness elliptical polarization.

To understand the phase difference between the TE and TM components of the surface wave, we write, in the local coordinate, the three components of the Poynting vector in the surrounding medium as

In the above equations, the y′ and z′ components of the Poyting vector are imaginary and real, respectively, regardless of the value of γ. However, to ensure that the x′ component of Poynting vector in the surrounding medium is real, γ needs to be real, i.e., there is a phase difference between TE and TM components. Further, we write the angle between phase velocity and group velocity as Intuitively, the angle between the phase velocity and the group velocity increases when the equifrequency contour of the surface wave deviates from a circular shape. Thus, θ decreases with the increase in εs as the EFC varies from concave to convex and approaches a circular shape. On the other hand, the ratio between the TE and TM components increases monotonously with θ for γ less than , as indicated by Equation (4). That is to say, a concave surface wave exhibits smaller ellipticity than the flat and concave surface waves.

Interestingly, in the simulation of the excitation of the surface wave, we observe very strong helicity-dependent directional surface wave excitation for the concave surface wave. Specifically, an incident light with circular polarization can preferably excite the surface wave along one specific direction or the other depending on the helicity of the incident wave. This arises from the direction-dependent helicity of the surface wave, which is verified by the full-wave simulation as shown in Figure 5. The surface wave is tilted to the right for the left circularly polarized (LCP) incidence, or to the left for the right circularly polarized (RCP) incidence, due to the matching of the helicity between the incident wave and the surface wave of oblique directions.

Figure 5
Figure 5

The simulation results of normalized electric field intensity under LCP excitation (a, b) and RCP excitation (c, d). The excited surface wave is tilted right and left for LCP and RCP, respectively. (a) and (c) show simulations with effective medium, while (b) and (d) show simulation results with realistic metamaterial structures.

Conclusion

In conclusion, we demonstrate a new kind of surface wave between a biaxial hyperbolic metamaterial and a normal isotropic dielectric. It is shown that the wave front of the surface wave is sensitively dependent on the refractive index of the surrounding medium. Almost flat k dispersion exists for certain refractive indexes of the surrounding medium, which could lead to highly compact self-guiding surface waves without adding nonlinearity or lateral confinements. The surface wave supported by a BHM shows an elliptically polarized state, whose ellipticity depends on the direction of propagation. Therefore, strong spin-orbital coupling is achieved in our system, which allows us to selectively control the wave propagation by the polarization handedness. These findings expand the horizon of nano optics based on surface waves, manifesting potential applications in both classical and quantum optical signal communication and processing.

References

  1. 1.

    . Surface Plasmons on Smooth and Rough Surfaces and on Gratings. Berlin: Springer-Verlag; 1988.

  2. 2.

    . Plasmonics: merging photonics and electronics at nanoscale dimensions. Science 2006; 311: 189–193.

  3. 3.

    , . Plasmonics: optics at the nanoscale. Mater Today 2005; 8: 56.

  4. 4.

    , , , , . Surface plasmon polaritons in generalized slab heterostructures with negative permittivity and permeability. Phys Rev B 2006; 73: 085104.

  5. 5.

    . Negative refraction makes a perfect lens. Phys Rev Lett 2000; 85: 3966–3969.

  6. 6.

    , , , . Sub–diffraction-limited optical imaging with a silver superlens. Science 2005; 308: 534–537.

  7. 7.

    , , , , . Near-field microscopy through a SiC superlens. Science 2006; 313: 1595.

  8. 8.

    , , , , et al. Biosensing with plasmonic nanosensors. Nat Mater 2008; 7: 442–453.

  9. 9.

    , , . Nano-optics from sensing to waveguiding. Nat Photonics 2007; 1: 641–648.

  10. 10.

    , , , , et al. Local detection of electromagnetic energy transport below the diffraction limit in metal nanoparticle plasmon waveguides. Nat Mater 2003; 2: 229–232.

  11. 11.

    , , , , . Channel plasmon subwavelength waveguide components including interferometers and ring resonators. Nature 2006; 440: 508–511.

  12. 12.

    , , , , . Plasmonic nanolithography. Nano Lett 2004; 4: 1085–1088.

  13. 13.

    , , , , et al. Focusing surface plasmons with a plasmonic lens. Nano Lett 2005; 5: 1726–1729.

  14. 14.

    , , . Mimicking surface plasmons with structured surfaces. Science 2004; 305: 847–848.

  15. 15.

    , , . Experimental verification of designer surface plasmons. Science 2005; 308: 670–672.

  16. 16.

    , , , , et al. Highly confined guiding of terahertz surface plasmon polaritons on structured metal surfaces. Nat Photonics 2008; 2: 175–179.

  17. 17.

    , , , . Ultrawide-bandwidth slow-light system based on THz plasmonic graded metallic grating structures. Phys Rev Lett 2008; 100: 256803.

  18. 18.

    , , , , et al. Helicity dependent directional surface plasmon polariton excitation using a metasurface with interfacial phase discontinuity. Light Sci Appl 2013; 2: e70; doi:10.1038/lsa.2013.26.

  19. 19.

    , , , , et al. Polarization-controlled tunable directional coupling of surface plasmon polaritons. Science 2013; 340: 331–334.

  20. 20.

    . New type of electromagnetic wave propagating at an interface. Sov Phys JETP 1988; 67: 714–716.

  21. 21.

    , . Dyakonov surface waves in photonic metamaterials. Phys Rev Lett 2005; 94: 013901.

  22. 22.

    , , , . Engineered surface waves in hyperbolic metamaterials. Opt Express 2013; 21: 19113–19127.

  23. 23.

    , . Optical hyperspace for plasmons: Dyakonov states in metamaterials. Appl Phys Lett 2008; 93: 221109.

  24. 24.

    , , . Optical hyperlens: far-field imaging beyond the diffraction limit. Opt Express 2006; 14: 8247–8256.

  25. 25.

    , . Far-field subdiffraction optical microscopy using metamaterial crystals: theory and simulations, Phys Rev B 2006; 74: 075103.

  26. 26.

    , , , . Guiding, focusing, and sensing on the subwavelength scale using metallic wire arrays. Phys Rev Lett 2007; 99: 053903.

  27. 27.

    , . Subwavelength imaging at optical frequencies using a transmission device formed by a periodic layered metal-dielectric structure operating in the canalization regime. Phys Rev B 2006; 73: 113110.

  28. 28.

    , , , , . Far-field optical hyperlens magnifying sub-diffraction-limited objects. Science 2007; 315: 1686.

  29. 29.

    , , . Magnifying superlens in the visible frequency range. Science 2007; 315: 1699–1701.

  30. 30.

    , , , , et al. Spherical hyperlens for two-dimensional sub-diffractional imaging at visible frequencies. Nat comm 2010; 1: 143.

  31. 31.

    , , . Broadband Purcell effect: radiative decay engineering with metamaterials. Appl Phys Lett 2012; 100: 181105.

  32. 32.

    , , , , et al. Control of spontaneous emission in a volume of functionalized hyperbolic metamaterial. Appl Phys Lett 2011; 99: 151115.

  33. 33.

    , , , . Enhancing spontaneous emission rates of molecules using nanopatterned multilayer hyperbolic metamaterials. Nat Nanotech 2014; 9: 48–53.

  34. 34.

    , , . Conical diffraction and the dispersion surface of hyperbolic metamaterials. Phys Rev A 2014; 90: 013803.

  35. 35.

    . Electromagnetic Mixing Formulas and Applications. London: Institution of Electrical Engineers; 1999.

  36. 36.

    , , , . Engineered surface waves in hyperbolic metamaterials. Opt Express 2013; 21: 19113–19127.

Download references

Acknowledgements

This work is supported by NSFC under Project 61328503 and the Leverhulme Trust (Grant No. RPG-2012-674). W. G thanks Chinese Scholarship Council Grant No. 201306250106.

Note: Accepted article preview online 9 May 2015

Author information

Affiliations

  1. State Key Laboratory of Precision Measuring Technology and Instruments, Tianjin University, Tianjin 300072, China

    • Wen-Long Gao
    • , Feng-Zhou Fang
    •  & Shuang Zhang
  2. School of Physics & Astronomy, University of Birmingham, Birmingham B15 2TT, UK

    • Wen-Long Gao
    •  & Shuang Zhang
  3. Department of Mechanical and Industrial Engineering, Northeastern University, Boston, MA 02115, USA

    • Yong-Min Liu
  4. Department of Electrical and Computer Engineering, Northeastern University, Boston, MA 02115, USA

    • Yong-Min Liu

Authors

  1. Search for Wen-Long Gao in:

  2. Search for Feng-Zhou Fang in:

  3. Search for Yong-Min Liu in:

  4. Search for Shuang Zhang in:

Corresponding authors

Correspondence to Yong-Min Liu or Shuang Zhang.

About this article

Publication history

Received

Revised

Accepted

Published

DOI

https://doi.org/10.1038/lsa.2015.101

Further reading