Abstract
Light reflection and refraction at an interface between two homogeneous media is analytically described by Snell's law. For a beam with a finite waist, it turns out that the reflected wave experiences a lateral displacement from its position predicted by geometric optics. Such GoosHänchen (GH) effect has been extensively investigated among all kinds of optical media, such as dielectrics, metals, photonic crystals and metamaterials. As a fundamental physics phenomenon, the GH effect has been extended to acoustics and quantum mechanics. Here we report the unusual GH effect in zero index metamaterials. We show that when linearly polarized light is obliquely incident from air to epsilonnearzero metamaterials, no GH effect could be observed for p polarized light. While for s polarization, the GH shift is a constant value for any incident angle.
Introduction
It is well known that when light is totally reflected from an interface of two media, it will experience a lateral displacement from the position predicted by the geometric optics. Such a lateral displacement is called the GoosHänchen (GH) shift^{1}. In the past few decades, the GH effect has been extensively explored in numerous interfaces involving absorptive dielectrics^{2,3,4}, metals^{5,6} and photonic crystals^{7,8,9}. Particularly, the total reflected wave undergoes a negative GH shift for a metamaterial with negative refractive index^{10}. Apart from total reflections, the GH effect has also been observed for partial reflections or transmissions at the interfaces^{4,11}. Due to its broad interest, the GH effect has also been extended to other physics systems, including nonlinear optics^{12}, acoustics^{13} and quantum mechanics^{14,15}. Several theoretical methods have been developed to understand the GH effect, such as stationary phase and energy propagation^{16,17}. For the stationary phase method, the GH shift can be given bywhere λ is the wavelength, ϕ(θ_{in}) is the phase of the reflected coefficient and θ_{in} is the incident angle.
Recently, zero index metamaterials (ZIMs) have drawn much attention for their intriguing electromagnetic (EM) properties^{18,19,20,21,22,23,24,25,26,27}. In particular, as a kind of ZIMs, the epsilonnearzero (ENZ) metamaterials has attracted more attention because they can be found in nature or be fabricated easily, e.g, the plasmonic materials at optical frequency^{28} or doped semiconductors at terahertz (THz) region^{29}. Nevertheless, to the best of our knowledge, there is no research on the GH effect in ZIMs. Generally, the GH shifts are positive among lossless dielectrics with a positive index, while they turn negative in lossless metamaterials with a negative index. It seems that the GH shifts should be zero in ZIMs. In this work, we will explore the GH effect when a linearly polarized light is obliquely incident from air onto an ENZ metamaterial. We decompose the linearly polarized light into two independent polarizations, i.e. the s polarized light with its electricfield vector perpendicular to the incident plane, and the p polarized light with its electricfield vector parallel to the incident plane. It is shown that there is no GH effect for p polarized light, while for s polarization, the GH shift is a constant value, independent of the incident angle. Such a unique behavior has not yet been revealed in previous study on the GH effect.
Results
Theoretical analysis
Our configuration is shown the schematically in Fig. 1. An interface in xy plane separates two semiinfinite media. Region 1 is air, and region 2 is ENZ metamaterial with parameters μ_{2} = 1 and ε_{2} ≈ 0 (we assume that the ENZ metamaterial is homogenous and isotropic). A linearly polarized light with incident angle θ_{in}_{ }is incident from air onto ENZ metamaterial. As known, the ENZ metamaterial can be regarded as optically thinner medium compared to air, and the critical angle for total reflection to occur is given by . As the permittivity of ENZ metamaterial is about zero, the critical angle tends to zero. Physically, the linearly polarized light, both s and p polarizations, will be totally reflected by the ENZ metamaterial for any incident angles excluding the normal one.
For GH effect, however, both polarizations have different responses during such a total reflection process. First, let us consider the s polarization. Suppose the incident linearly polarized light with an angular frequency ω is given as , where k_{x} = k_{0} sin θ_{in}, k_{z} = k_{0} cos θ_{in}, and k_{0} = ω/c is the wave number in air, c is the velocity of light in air. For simplicity, the time dependence exp(−iωt) will be omitted throughout this work. After reflection by ENZ metamaterial, the reflected light is . Inside region 2 of ENZ metamaterial, the refracted light is expressed as , where . In addition, each corresponding magnetic field can be calculated from one of Maxwell's equations . Applying the continuous boundary conditions of tangential electric and magnetic fields at z = 0, the reflected coefficient is calculated as with its phase, By employing the method of stationary phase as shown by the equation (1), the GH shift can be achieved asIt is noted that this result is not valid at 90°, as the equation (1) for quantitatively analyzing the GH shift is not defined there^{10}. From equation (4), it is obviously seen that when the permittivity ε_{2} is close to zero, i.e. ε_{2} ≈ 0, the GH shift is d_{s} = λ/π, a constant value for any incident angle. Meanwhile, we can work out that the phase of reflected light is ϕ_{s} = −2θ_{in} from equation (2), which is a linear function of the incident angle.
A similar procedure can be implemented for p polarized light. In this case, electricfield in y direction in the above equations should be changed into magnetic field. In region 1 of air, the incident and reflected light can be written as and , respectively. In the region of ENZ metamaterial, the refracted light is . Similarly, the corresponding electric fields could be obtained by one of the Maxwell's equations . Applying the continuous boundary conditions, the reflected coefficient is calculated as with its phase expressed asApplying the same method of equation (1), the GH shift for p polarized light is given as From this equation (7), we know that for the ENZ metamaterial with the permittivity ε_{2} ≈ 0, the GH shift is d_{p} = 0 for any incident angle. From equation (6), the phase of reflected light is −π, which means there is a halfwave phase lag for p polarized light after total reflection. Such a feature is analogous to the propagation of the s polarized light reflected by the perfect electric metal. With that in mind, the ENZ metamaterial could be regarded as a perfect magnetic conductor (PMC) for p polarized light. From the perspective of intrinsic property of ENZ metamaterial, we know that as the permittivity ε_{2} tends to zero, the right term in Maxwell's Equation should vanish, in order to keep a finite value of electric field. As a result, the magnetic field inside the ENZ material should be a constant^{25}, that is H_{2} = Const. Then, following the continuous conditions of the magnetic fields at the boundary z = 0, we get (H^{r} + H)exp(ik_{x}x) = Const. For the p polarized light obliquely incident onto the ENZ material, we have k_{x} ≠ 0. To keep the above boundary condition valid for arbitrary coordinate x, the only satisfaction is that H^{r} + H = 0. It also means that the magnetic field inside ENZ metamaterial is exactly zero. Consequently, the reflected coefficient is ρ_{p} = H^{r}/H = −1 and its reflected phase is −π. Such understanding from the intrinsic property itself is more straightforward, and gives the same results on GH effect for p polarized light.
The GH effect can also be interpreted from the point of view of an energy flow along the interface in the optically thinner medium^{16} (e.g. the ENZ metamaterial). The time averaged energy flow can be calculated by applying (the star sign represents the conjugate operation). For s polarized incident light, we have and . Moreover, the penetrated length could be defined by l = 1/κ. It implies that the incident EM energy will enter into ENZ metamaterial, and the energy will go back into air when it arrives at z = l. Moreover, the GH shift from the view of geometric optics, is d ≈ 2l sin θ_{in} = λ/π when ε_{2} ≈ 0. For p polarized light, however, the corresponding averaged energy flow is because the magnetic field inside ENZ material is exactly zero. It means that no electromagnetic energy enters into ENZ metamaterial, thereby leading to no GH effect. This view from the surface energy flow further corroborated our analysis.
Influence of losses
We considered a lossless ENZ metamaterial in above theoretical analysis. However, for a real ENZ metamaterial, such as the noble metal at plasma frequency or doped semiconductors at terahertz^{28,29}, their losses should be considered. In the following, we will illustrate the influence of loss on the GH shifts for s and p polarized light. For an absorptive medium, the equation (1) quantifying the GH shift should be rewritten as (m = s and p)^{30}, where the prime indicates the derivative with respect to θ_{in}. Combining equation (2) and equation (5), the GH shifts for two polarizations are given as,when Im[ε_{2}] ≠ 0, where Re[ε_{2}] and Im[ε_{2}] represent, respectively, the real part and imaginary part of the permittivity of loss ENZ metamaterial. As usual, the imaginary part indicates the loss.
Based on the above formulas, Fig. 2 shows the calculated GH shifts for different values of the loss parameter of ENZ metamaterials. In Fig. 2a, we set Re[ε_{2}] = 10^{−4}, and the solid and dashed lines are corresponding to s and p polarizations, respectively. As shown by the blue lines, the GH shifts for both polarized light of s and p are d_{s} = λ/π and d_{p} = 0, respectively, for any incident angle except the vicinity of the critical angle. It is noted that when the incident angles vary across the critical one, the reflection phase will experience an abrupt change, usually leading to quite an obvious GH effect^{31}. When the loss is taken into account, e.g. Im[ε_{2}] = 0.01, for s polarized light, as shown by the black solid line, there is a region where the GH shift gradually changes from zero to λ/π. Such a property stems from the fact that the added losses make the reflection phases deviate from the linear relationship of ϕ_{s} = −2θ_{in}. In particular, the deviation is quite notable at small incident angle. For p polarized light, however, the situation is more complicated. Generally, for an absorptive medium, there is an abrupt change of phase across the (pseudo) Brewster angle when a p polarized light is reflected by it. As a result, such an abruptly changed phase induces a negative GH shift around the (pseudo) Brewster angle^{3}. It is also true for lossy ENZ metamaterials. For instance, when the loss is Im[ε_{2}] = 0.01, as shown by the black dashed line, a resonance for GH shift could be observed. Further, we use a larger loss with Im[ε_{2}] = 0.1, as shown by the red lines. The gradually changing region of GH shift for s polarized light is enlarged (see the red solid line), while for p polarized light, the resonance position is shifted to a larger angle (see the red dashed line). Nevertheless, for an incident angle large enough, the GH shifts for the loss cases will approach those of the situation without loss, i.e., for s polarized light, it is almost λ/π, while for p polarized light, it is close to zero. The larger the loss is, the narrower the range of the working incident angle is. In particular, the working incident angle range for Im[ε_{2}] = 0.01 is at about [15°, 90°), while for Im[ε_{2}] = 0.1, it changes into [40°, 90°).
In order to examine the sensitivity of the small values of Re[ε_{2}] to the GH shift, Fig. 2b shows the calculated results when Re[ε_{2}] increases to 10^{−2}. For the lossless case, the critical angle becomes larger, then the working angle for both polarizations is accordingly shifted to a larger angle, as shown by the blue lines. When the same levels of losses are involved, the black and red lines are corresponding to those of Im[ε_{2}] = 0.01 and 0.1, respectively. Similar results can be observed including the gradually changed regions of GH shifts for s polarized light and the resonances of GH shifts for p polarized light. Although the real part of the permittivity is larger, the working incident angle ranges do not vary that much if we compare Fig. 2a and Fig. 2b. For the same loss, the positions of resonances are shifted very slightly when the Re[ε_{2}] increases from 10^{−4} to 10^{−2}. However, the amplitudes of resonances change a little bit. Generally, for an absorptive dielectric, the amplitudes of resonances decrease as the ratio of Im[ε_{2}]/Re[ε_{2}] increases^{30}. For the ENZ metamaterials with different losses, the amplitudes of resonances have the same tendency.
Numerical simulations
To give a comprehensive understanding and to verify the above theoretical analysis, we perform the numerical simulations of GH shifts, where we consider a beam with a spatial Gaussian profile incident from air to ENZ metamaterial, and the halfwidth of the beam is 7.5λ. Because of the small GH shift, it is easier to observe the lateral shift L = d_{s}/cos(θ_{in}). Fig. 3 shows the simulated results when the incident angle is 45°, in which for s polarization, the lateral shift L is about 0.5λ, as shown in Fig. 3a, while for p polarization, the shift is zero, as shown in Fig. 3b. Theoretically, the value is about 0.45λ for spolarization. Considering the fact that the incident beam is not a plane wave, such a deviation is acceptable. Moreover, Fig. 3c shows the distributions of field amplitude near the interfaces for two polarizations, as shown by the red line and the black dashed line respectively. It is clearly seen that for p polarization, the symmetry axis of the field distribution (the red line) is located at the original point x = 0, as shown by the dotted line. While for s polarization its symmetric center is shifted to the left. Such a contrast further verifies our theoretical prediction that the GH shift exists only for s polarization. Lastly, we compare the numerical results L for different incident angles with the analyzed results, as shown in Fig. 3d. The black line is given by the formula L = d_{s}/cos(θ_{in}), while the five blue points are the numerical results for incident angles with 15°, 30°, 45°, 60° and 75°, respectively. In the plot, the numerical results fit well with the analytical curve.
Finally, it is worth mentioning that we only focus on the ENZ metamaterials here. In fact, the zero index metamaetrials can be further categorized, e.g., munearzero (MNZ) metamaterials, matched impedance zeroindex metamaterials (MIZIMs), and anisotropic ZIMs. For MNZ metamaterials, we predict based on current results that the GH shift is a constant for p polarized light, independent of the incident angle. Yet, there is no GH shift for s polarization. For MIZIMs, there are no GH shifts for both polarizations of s and p because the oblique incident light cannot enter into MIZIMs at all.
Discussion
We have investigated the GH effect of reflected light, when a linearly polarized light of either s or p polarization is obliquely incident onto the ENZ metamaterial from air. We have shown that for lossless ENZ material, there is no GH shift for p polarization, which indicates that it obeys exactly the prediction by the geometrical optics. While for s polarization, the GH shift is a constant value, independent of the incident angle. We also have explored analytically the influence of loss of ENZ metamaterials on the GH shift for both polarizations and we found that the novel features still hold for a broad range of angles. Analogous deviations of GH effect are expected for acoustic waves, quantum matter waves and so on. In addition, we have shown that the reflected phase of p polarized light is ϕ_{p} = −π, while for p polarized light, the reflected phase obeys that linear relationship ϕ_{s} = −2θ_{in}. Due to such different responses, we believe that the ENZ metamaterial can be utilized to manipulate the polarization states of reflected light, by only adjusting the incident angle. We expect our work to contribute some new notions to the manipulation of the polarization states of light at the THz region.
Methods
Theory and simulations
The numerical simulation results shown in Fig. 3a and 3b were obtained using the finite element solver COMSOL Multiphysics. The scattering boundaries were set for four sides. Based on these numerical simulations, the curves of field amplitudes in Fig. 3c were obtained by performing the line plot along x axis from −8λ to 8λ. Due to the interference effect, the field amplitudes are oscillating along z direction. The line plots are located at the first peak close to the interface between air and ENZ metamaterial. Meanwhile, we zoom in the line plot of E_{y} enough to get the distance between its symmetric axis and x = 0, which indicates the lateral shift L. The numerical results in Fig. 3d were obtained by the same technique.
References
 1.
Goos, F. & Hänchen, H. Ein neuer und fundamentaler Versuch zur Totalreflexion. Ann. Phys. 436, 333–346 (1947).
 2.
Wild, W. J. & Giles, C. L. GoosHänchen shifts from absorbing media. Phys. Rev. A 25, 2099 (1982).
 3.
Lai, H. M. & Chan, S. W. Large and negative Goos–Hänchen shift near the Brewster dip on reflection from weakly absorbing media. Opt. Lett. 27, 9 (2002).
 4.
Wang, L. G., Chen, H. & Zhu, S. Y. Large negative Goos–Hänchen shift from a weakly absorbing dielectric slab. Opt. Lett. 30, 2936 (2005).
 5.
Leung, P. T., Chen, C. W. & Chiang, H. P. Large negative GoosHänchen shift at metal surfaces. Opt. Commum. 276, 206–208 (2007).
 6.
Merano, M. et al. Observation of GoosHänchen shifts in metallic reflection. Opt. Express 15, 15928 (2007).
 7.
Felbacq, D., Moreau, A. & Smâli, R. GoosHänchen effect in the gaps of photonic crystals. Opt. Lett. 28, 1633–1635 (2003).
 8.
He, J., Yi, J. & He, S. Giant negative GoosHänchen shifts for a photonic crystal with a negative effective index. Opt. Express 14, 3024 (2006).
 9.
Soboleva, I. V., Moskalenko, V. V. & Fedyanin, A. A. Giant GoosHänchen effect and Fano resonance at photonic crystal surfaces. Phys. Rev. Lett. 108, 123901 (2012).
 10.
Berman, P. R. GoosHänchen shift in negatively refractive media. Phys. Rev. E 66, 067603 (2002).
 11.
Li, C. F. Negative lateral shift of a light beam transmitted through a dielectric slab and interaction of boundary effects. Phys. Rev. Lett. 91, 133903 (2003).
 12.
Emile, O., Galstyan, T., Floch, A. & Bretenaker, F. Measurement of the nonlinear GoosHänchen effect for Gaussian optical beams. Phys. Rev. Lett. 75, 1511 (1995).
 13.
Briers, R., Leroy, O. & Shkerdin, G. Bounded beam interaction with thin inclusions. Characterization by phase differences at Rayleigh angle incidence. J. Acoust. Soc. Am. 108, 1622 (2000).
 14.
Beenakker, C. W. J., Sepkhanov, R. A., Akhmerov, A. R. & Tworzydło, J. Quantum GoosHänchen effect in graphene. Phys. Rev. Lett. 102, 146804 (2009).
 15.
de Haan, V. O. et al. Observation of the GoosHänchen shift with neutrons. Phys. Rev. Lett. 104, 010401 (2010).
 16.
Chiu, K. W. & Quinn, J. J. On the GoosHänchen effect: A simple example of time delay scattering process. Am. J. Phys. 40, 1847 (1972).
 17.
Renard, R. H. Total reflection: A new evaluation of the GoosHänchen shift. J. Opt. Soc. Am. 54, 1190 (1964).
 18.
Silveirinha, M. & Engheta, N. Tunneling of electromagnetic energy through subwavelength channels and bends using εnearzero materials. Phys. Rev. Lett. 97, 157403 (2006).
 19.
Alù, A., Silveirinha, M. G., Salandrino, A. & Engheta, N. Epsilonnearzero metamaterials and electromagnetic sources: Tailoring the radiation phase pattern. Phys. Rev. B 75, 155410 (2007).
 20.
Silveirinha, M. & Engheta, N. Theory of supercoupling, squeezing wave energy, and field confinement in narrow channels and tight bends using εnearzero metamaterials. Phys. Rev. B 76, 245109 (2007).
 21.
Edwards, B., Alù, A., Young, M. E., Silveirinha, M. & Engheta, N. Experimental verification of epsilonnearzero metamaterial coupling and energy squeezing using a microwave Waveguide. Phys. Rev. Lett. 100, 033903 (2008).
 22.
Liu, R. et al. Experimental demonstration of electromagnetic tunneling through an epsilonnearzero metamaterial at microwave frequencies. Phys. Rev. Lett. 100, 023903 (2008).
 23.
Hao, J., Yan, W. & Qiu, M. Superreflection and cloaking based on zero index metamaterial. Appl. Phys. Lett. 96, 101109 (2010).
 24.
Nguyen, V. C., Chen, L. & Halterman, K. Total transmission and total reflection by zero index metamaterials with defects. Phys. Rev. Lett. 105, 233908 (2010).
 25.
Xu, Y. & Chen, H. Total reflection and transmission by epsilonnearzero metamaterials with defects. Appl. Phys. Lett. 98, 113501 (2011).
 26.
Huang, X., Lai, Y., Hang, Z. H., Zheng, H. & Chan, C. T. Dirac cones induced by accidental degeneracy in photonic crystals and zerorefractiveindex materials. Nat. Mater. 10, 582–586 (2011).
 27.
Chan, C. T., Huang, X. Q., Liu, F. & Hang, Z. H. Dirac dispersion and zeroindex in two dimensional and three dimensional photonic and phononic systems. Progress In Electromagnetics Research B 44, 163–190 (2012).
 28.
Wes, P. R. et al. Searching for better plasmonic materials. Laser Photon. Rev. 4, 6 (2010).
 29.
Adams, D. C. et al. Funneling light through a subwavelength aperture with epsilonnearzero materials. Phys. Rev. Lett. 107, 133901 (2011).
 30.
Götte, J. B., Aiello, A. & Woerdman, J. P. Lossinduced transition of the GoosHänchen effect for metals and dielectrics. Opt. Express 16, 3961 (2008).
 31.
Schwefel, H., Köhler, W., Lu, Z., Fan, J. & Wang, L. Direct experimental observation of the single reflection optical Goos–Hänchen shift. Opt. Lett. 33, 794–796 (2008).
Acknowledgements
This work was supported by the National Science Foundation of China for Excellent Young Scientists (grant no. 61322504), the National Excellent Doctoral Dissertation of China (grant no. 201217), the National Natural Science Foundation of China (grant No. 11004147) and the Priority Academic Program Development (PAPD) of Jiangsu Higher Education Institutions. C.T.C. was support by RGC grants 600311 and AOE/P02/12.
Author information
Affiliations
College of Physics, Optoelectronics and Energy, Soochow University, No.1 Shizi Street, Suzhou 215006, China
 Yadong Xu
 & Huanyang Chen
Department of Physics and Institute for Advanced Study, Hong Kong University of Science and Technology, Clear Water Bay, Hong Kong, China
 C. T. Chan
Authors
Search for Yadong Xu in:
Search for C. T. Chan in:
Search for Huanyang Chen in:
Contributions
Y.X. and H.C. conceived the idea. Y.X. did the theoretical calculations and the numerical simulations. H.C. and C.T.C. helped with the theoretical analysis. H.C. supervised the whole project. All the authors wrote the manuscript.
Competing interests
The authors declare no competing financial interests.
Corresponding author
Correspondence to Huanyang Chen.
Rights and permissions
This work is licensed under a Creative Commons Attribution 4.0 International License. The images or other third party material in this article are included in the article's Creative Commons license, unless indicated otherwise in the credit line; if the material is not included under the Creative Commons license, users will need to obtain permission from the license holder in order to reproduce the material. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/
About this article
Further reading

Asymmetric effects in waveguide systems using PT symmetry and zero index metamaterials
Scientific Reports (2017)

Magnetic control of GoosHänchen shifts in a yttriumirongarnet film
Scientific Reports (2017)

GoosHänchen shift of partially coherent light fields in epsilonnearzero metamaterials
Scientific Reports (2016)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.