## Abstract

We design an all–dielectric Lüneburg lens as an adiabatic space–variant lattice explicitly accounting for finite film thickness. We describe an all–analytical approach to compensate for the finite height of subwavelength dielectric structures in the pass–band regime. This method calculates the effective refractive index of the infinite–height lattice from effective medium theory, then embeds a medium of the same effective index into a slab waveguide of finite height and uses the waveguide dispersion diagram to calculate a new effective index. The results are compared with the conventional numerical treatment – a direct band diagram calculation, using a modified three–dimensional lattice with the superstrate and substrate included in the cell geometry. We show that the analytical results are in good agreement with the numerical ones, and the performance of the thin–film Lüneburg lens is quite different than the estimates obtained assuming infinite height.

© 2012 OSA

## 1. Introduction

Gradient Index (GRIN) media have been known to offer rich possibilities for light manipulation since at least Maxwell’s time [1]. More recent significant examples are the Lüneburg lens [2], the Eaton lens [3], and the plethora of imaging and cloaking configurations devised recently using conformal maps and transformation optics [4–8]. GRIN optics are of course also commercially available, but the achievable refractive index profiles *n*(**r**) are limited generally to parabolic in the lateral coordinates or to axial without any lateral dependence [9]. There is an ongoing effort to achieve more general distributions using stacking of photo-exposed polymers [10, 11].

For optics-on-a-chip or integrated optics applications, it is possible to *emulate* an effective index distribution *n*(**r**) by patterning a substrate with subwavelength structures. If these are sufficiently smaller than the wavelength, to a good approximation they can be thought of as a continuum where the effective index is determined by the pattern geometry. For example, one can create a lattice of alternating dielectric–air with slowly varying period and fixed duty cycle, or with fixed period but slowly varying duty cycle [12, 13].

If the critical length of the variation is slow enough compared to the lattice constant that the adiabatic approximation is valid, the lattice dispersion diagram can be used to estimate the local effective index [12,13]. Refractive indices computed using a 2D approximation are valid for 2D adiabatically variant metamaterials where the height in the 3^{rd} dimension is much larger than the wavelength so the assumption of infinite height can be justified. According to this, we have designed a subwavelength aperiodic nanostructured Lüneburg lens [14,15]. This lens mimics a GRIN element with refractive index distribution
$n\left(\rho \right)={n}_{0}\sqrt{2-{\left(\rho /R\right)}^{2}}$ (0 < *ρ* < *R*), where *n*_{0} is the ambient index outside the lens region, *R* is the radius of the lens region and *ρ* is the radial polar coordinate with the lens region as origin. The Lüneburg lens focuses an incoming plane wave from any arbitrary direction to a geometrically perfect focal point at the opposite edge of the lens [2, 16].

However, most such adiabatically variant structures are fabricated by etching holes or rods on a thin silicon film, whose height is less than even the optical wavelength [6, 14, 15, 17, 18]. Hence, the infinite height assumption becomes questionable. Moreover, the structures are asymmetric since typically beneath the structure there is a substrate such as glass, whereas above the structure is air. Asymmetry also induces a long–wavelength cutoff in the guided modes [19]; therefore the thin–film metamaterial should operate in an intermediate regime where the wavelength is neither too large nor too small. The problem of asymmetry and finite height have been acknowledged in the literature on photonic crystals [20–24], where the most common solution is to compute a full 3D band diagram [25]. Most of them focus on photonic crystal slabs operating at wavelengths comparable to the periodicity, discussing phenomena such as super–collimation [26], negative refraction [27], etc. To the best of our knowledge, the same problem has received insufficient attention in the context of 2D dielectric periodic or aperiodic metamaterial devices, especially those operating at the propagation regime of the band diagram. It has been briefly mentioned in [6, 28] without giving a detailed solution.

In our fabricated Lüneburg lens design, thin–film problem is obvious where the experimental results show dislocated and aberrated focal point [14, 15]. In this paper we re–designed the Lüneburg lens to include the finite film thickness, improving the estimate of the expected focal point position. To design such a lens, first we need a method for estimating effective refractive index of thin–film metamaterials. Several methods have been proposed in the literature. A conventional numerical approach (we refer to it as Direct Band Diagram, DBD) in photonic crystals derives a 3D lattice cell from the original 2D cell by surrounding a finite–height rod with large spaces of air above and glass substrate below [25]. Another method takes one unit cell and retrieve the refractive index by its reflection and refraction properties [29]. These methods yield accurate results but require either 3D band or finite–difference calculations. More heuristic (but faster) effective–index methods estimate a slab–waveguide effective index first and then use it to compute a 2D band diagram or effective index [30]. They are generally suitable for structures with etched substrates. In contrast, our proposal essentially reverses the order of these steps: we compute an effective index from the 2D cross–section first, and then incorporate it into a slab–waveguide mode. This is more suitable to the metamaterial regime.

In particular, we propose the following all–analytical method for effective refractive index calculation. First, we replace the rods with a continuum of a certain effective permittivity ${\varepsilon}_{\text{eff}}^{2\text{D}}$. We calculate ${\varepsilon}_{\text{eff}}^{2\text{D}}$ from 2D lattice of infinite–height rods using second-order effective medium theory, and then substitute ${\varepsilon}_{\text{eff}}^{2\text{D}}$ as the permittivity of a slab of finite thickness, acting as an effective guiding medium, sandwiched between semi-infinite spaces of air above and glass below. The geometry then becomes one of a weakly–guiding waveguide due to the small height of the effective guiding medium. This weakly–guiding effect modifies the real part of the horizontal wave–vector component, and thus a new effective permittivity ${\varepsilon}_{\text{eff}}^{3\text{D}}$ for the finite slab of rods is derived from the waveguide dispersion relationship. We refer to this method as Effective Guiding Medium (EGM). Comparing with rigorous 3D calculations, our method provides more physical insights, and is generally faster to compute.

To validate our method, we compare it with the DBD method. It is shown that the results of both methods are in good agreement.

## 2. Analytical method for effective refractive index estimation

In this paper, without loss of generality, we investigate a silica glass slab covered by a square lattice (lattice constant *a* = 258 nm) of silicon rods of finite height *h* = 320 nm, variable radius
$r\left(0<r<a/\sqrt{2}\right)$ and immersed in air, as illustrated in Fig. 1(a). The free space wavelength of light is chosen as *λ* = 6*a* = 1550 nm. This choice of *a* is small enough to insure that we remain in the metamaterial regime and in the propagating regime of the band diagram; and large enough that the rods can be accurately fabricated by nano–lithography [14, 15] and we do not reach the long–wavelength cutoff regime for the asymmetric waveguide, as mentioned above. The dielectric permittivity constants for glass and silicon are *ɛ*_{glass} = 2.25 and *ɛ*_{silicon} = 12.0, respectively. These media are non–magnetic, so the relative permeability is taken as *μ* = 1 throughout this paper. The glass slab height is assumed to be much larger than the height of the rods and the free space wavelength of the light. The corresponding 2D structure with infinite height rods and without glass substrate is shown in Fig. 1(b). We now proceed to describe all–analytical method, EGM, for analyzing these two geometries.

#### 2.1. Effective guiding medium (EGM) method

The EGM method requires analysis of a three–layer structure: (I) air, (II) effective medium waveguide and (III) glass, as shown in Fig. 2. The effective permittivity of the guiding medium is calculated from the second–order effective medium theory in 2D which have been derived by various authors [31, 32]. This theory starts from the effective refractive index of 1D subwavelength grating composed of air and dielectric with index *n*. Under TE (electric field parallel to the grooves) and TM (electric field vertical to the grooves) polarization incidence the effective index can be summarized, respectively, as [32, 33]

*T*is the period of the grating and

*f*is the filling factor of the dielectric grooves. The effective indices of corresponding 2D subwavelength structures are then estimated as a combination of 1D structures [32, 33]

*λ*= 6

*a*used in this paper. Most current metamaterial device designs are using the zeroth–order approximation only [6], even when the unit cell size is not far smaller than the operational wavelength. This is fine for those devices where high accuracy results are not important. However, for devices such as Lüneburg lens, all waves are focusing to a single point so light manipulation is more challenging. Therefore, more precise effective index prediction is needed and second–order corrections are included.

The dispersion relation of the effective guiding medium, i.e. the relationship between *k _{z}* and

*ω*, is governed by the guidance condition of an asymmetric dielectric waveguide for both TE and TM polarizations [34]

*k*(

_{z}*ω*) are shown in the following section.

The EGM method described above is compared with the conventional DBD method. To apply the DBD method, we need to calculate the band diagram of the 3D super cell shown in Fig. 4(a). The supercell height is taken as large as *H* = 20*a* to better emulate the real structure of Fig. 1(a), where the air and glass spaces tend to infinity. In other words, we seek to minimize the interference between neighboring unit cells along the vertical (*y*) direction. We used the MIT Photonic–Bands (MPB) mode solver [35] to calculate the dispersion diagram. In Figs. 4(b)–4(c) we show an example MPB result for our chosen lattice and the specific value *r* = 0.5*a*, for temporal frequency *ω* = 1/6×2*πc/a*. From Fig. 4(b) we observe that for the chosen values of *r* and *ω*, the isofrequency contour [25] is almost a circle, indicating that this unit cell is isotropic. Therefore, when using DBD in this particular geometry, it is sufficient to consider *k _{z}*(

*ω*) only. However, this is not generally true in other geometries as

*r*or

*ω*increase.

Figure 4(c) shows the mode shape for the same geometry. It can be seen that the field is effectively concentrated near the silicon rod portion of the cell. The relative intensities at two horizontal cell boundaries *y* = ±*H*/2 were 5.6 × 10^{−6} and 3.8 × 10^{−6} at the top and bottom, respectively, compared to the peak value that occurred at *y* = 159 nm from the rod base. This validates our choice of *H* as sufficiently large.

Comparing with the DBD method, the EGM method can provide deeper physical insights with all–analytical solutions, and is generally faster since it avoids solving numerical electromagnetic solutions in 3D.

#### 2.2. Effective refractive index and rod radius relationship

In this section, the relationship between the effective refractive index and rod radius is calculated. The results of EGM method are compared with the ones obtained from DBD method.

Figure 5(a) shows the dispersion relation of the finite–height rod lattice calculated with both DBD and EGM methods, as well as with the 2D (infinite rod height) assumption, for rod radius *r* = 0.5*a*. Based on the dispersion relation, effective refractive indices for unit cells with different rod radii are calculated as *n*_{eff} = *ck _{z}*/

*ω*, shown in Fig. 5(b). The results given by the DBD and EGM methods are in good agreement with each other, with maximum percentage errors of 7.3% and 6.0% for 2D and 3D cases, respectively. It is observed that the effective refractive indices of the finite–height rods are significantly different than those assuming infinite height. This is to be expected due to weak guidance: as can been seen in Fig. 4(c), a large portion of the field extends outside the rods to spaces of air and substrate. When the rod radii are below certain values (0.17

*a*for TE and 0.35

*a*for TM), the propagation modes are not guided so the effective indices are not shown. The discontinuities observed in the 2D effective index curves for DBD method beyond certain values of rod radii (0.40

*a*for TE and 0.49

*a*for TM) result from the emergence of a photonic crystal bandgap at these values. At this frequency range, even though the 2D infinite–height lattice is within the bandgap, the confined (slab waveguide) geometry is still propagating; this is because the light is mostly outside the dielectric region, so propagation takes place in the free space (hence the lower index). To calculate the propagation constant in this regime, we still need an effective index value and EGM provides it (it turns out to be large than 3, typically).

## 3. Optimal design of the subwavelength Lüneburg lens

We re–design and numerically verify the subwavelength Lüneburg lens [2,14,15,36], which was previously designed under 2D assumption. Here, we still design the Lüneburg lens as a structure consisting of finite–height rods with adiabatically changing radius *r* across the lattice of fixed constant *a*. At each coordinate *ρ*, we emulate the Lüneburg distribution
$n\left(\rho \right)={n}_{0}\sqrt{2-{\left(\rho /R\right)}^{2}}$by choosing the rod radius *r* at coordinate *ρ* from Fig. 5(b) such that
${n}_{\text{eff}}^{3\text{D}}=n\left(\rho \right)$, as opposed to using
${n}_{\text{eff}}^{2\text{D}}=n\left(\rho \right)$. The design has to be carried out separately for the TE and TM polarizations. The ambient index is chosen as *n*_{0} = 1.53.

Figure 6 illustrates the lens structures and the corresponding 3D finite–difference time–domain (FDTD) simulation results for the actual adiabatically variant thin–film nanostructured Lüneburg lens performed by MIT Electromagnetic Equation Propagation (MEEP) [37]. The 3D model used for FDTD consists of a rectangular box of size 41*a*×24*a*×41*a* which contains perfectly matched layers on both sides of each dimension. The radius of the lens is chosen as 15*a*. With plane wave illumination, almost diffraction–limited focal points at the edge can be observed for both TE and TM polarizations. For a more computationally efficient and intuitive representation we also ray–traced the field inside the Lüneburg structure using the adiabatic Hamiltonian method [12, 13]. The ray position **q** and momentum **p** are obtained by solving the two sets of coupled ordinary differential equations

*H*(

**q**,

**p**) ≡

*ω*(

*ρ*,

**k**) is obtained from the dispersion diagram at each coordinate |

**q**| =

*ρ*and for

**k**≡

**p**. Ray tracing results are superimposed in Fig. 6 with FDTD results, and are seen to be in good agreement. Furthermore, as a comparison, similar thin–film Lüneburg lens is designed using the DBD method and simulation results are shown in Fig. 7. It is observed that results of the all–analytical EGM method design agree with those from the DBD method.

In Section 2.1 we mentioned the second–order effective medium theory for better approximation of the effective index when the wavelength is not significantly larger than the size of unit cell. To illustrate the importance of these second–order terms, we designed a thin–film Lüneburg lens using the EGM method, but the second–order terms were neglected when estimating the effective indices. The FDTD and ray–tracing results are shown in Fig. 8. The performance of the lens is degraded with aberrations and shifted focal position. Note that to clearly illustrate the focal points, we extended the size of the 3D FDTD model in *z* direction to 61*a*.

To compare the redesigned lens (3D, finite height) with the original design (2D, infinite height), we repeated the design using the values of refractive indices predicted by the dispersion relation of the infinite–height rod lattice (see Fig. 5(b) blue and red solid curves). In this case, we are forced to use TM polarization only because the TE polarization reaches the bandgap for relatively small value of *r*, not leaving enough room to implement the Lüneburg profile with rod radius *r* large enough to be robust to practical lithography and etching methods (in our experiment, this requires *r* ≥ 0.27*a* [14, 15]). Also, for better illustration, the size of 3D FDTD model is modified to 41*a* × 24*a* × 101*a*. It can be observed from the FDTD and Hamiltonian ray–tracing results shown in Fig. 9 that the focal point is outside the lens edge and it is strongly aberrated. This is in good agreement with the experimental results of the original design [14, 15].

## Acknowledgments

The authors thank Lei Tian for useful discussions and Justin W. Lee for setting up the computation server. Financial support was provided by Singapore’s National Research Foundation through the Singapore–MIT Alliance for Research and Technology (SMART) Centre and the Air Force Office of Scientific Research MURI program on Nanomembranes under contract No. FA9550-08-1-0379.

## References and links

**1. **C. A. Swainson (alias J. C. Maxwell), “Problems,” Cambridge Dublin Math. J. **8**, 188–189 (1854).

**2. **R. K. Lüneburg, *Mathematical Theory of Optics* (Brown U. P., 1944).

**3. **J. E. Eaton, An Extension of the Luneburg–Type Lenses (Rep. No. 4110, Naval Res. Lab., 1953).

**4. **U. Leonhardt, “Optical conformal mapping,” Science **312**, 1777–1780 (2006). [CrossRef] [PubMed]

**5. **J. B. Pendry, D. Schurig, and D. R. Smith, “Controlling electromagnetic fields,” Science **312**, 1780–1782 (2006). [CrossRef] [PubMed]

**6. **J. Valentine, J. Li, T. Zentgraf, G. Bartal, and X. Zhang, “An optical cloak made of dielectrics,” Nat. Mater. **8**, 568 (2009). [CrossRef] [PubMed]

**7. **D. H. Spadoti, L. H. Gabrielli, C. B. Poitras, and M. Lipson, “Focusing light in a curved-space,” Opt. Express **18**, 3181–3186 (2010). [CrossRef] [PubMed]

**8. **B. Vasić, G. Isić, R. Gajić, and K. Hingerl, “Controlling electromagnetic fields with graded photonic crystals in metamaterial regime,” Opt. Express **18**, 20321–20333 (2010). [CrossRef]

**9. **E. Hecht, *Optics*, (4th ed., Section 6.4) (Addison-Wesley, 2002).

**10. **G. R. Schmidt, *Compound Optical Arrays and Polymer Tapered Gradient Index Lenses (PhD Thesis)* (University of Rochester, 2009).

**11. ***Manufacturable Gradient Index Optics (M–GRIN)* (Broad Agency Announcement, Defense Advanced Research Projects Agency, 2010).

**12. **Y. Jiao, S. Fan, and D. A. B. Miller, “Designing for beam propagation in periodic and nonperiodic photonic nanostructures: Extended Hamiltonian method,” Phys. Rev. E **70**, 036612 (2004). [CrossRef]

**13. **P. S. J. Russel and T. A. Birks, “Hamiltonian optics of nonuniform photonic crystals,” J. Lightwave Technol. **17**, 1982–1988 (1999). [CrossRef]

**14. **S. Takahashi, C. Chang, S. Y. Yang, and G. Barbastathis, “Design and fabrication of dielectric nanostructured Luneburg lens in optical frequencies,” in Optical MEMS and Nanophotonics, (IEEE Photonics Society, 2010), Paper Th1–1. [CrossRef]

**15. **S. Takahashi, *Design and Fabrication of micro- and nano-dielectric structures for imaging and focusing at optical frequencies (PhD Thesis)* (Massachusetts Institute of Technology, 2011). [PubMed]

**16. **A. Vakil and N. Engheta, “Transformation optics using graphene,” Science **332**, 1291–1294 (2011). [CrossRef] [PubMed]

**17. **H. Gabrielli, J. Cardenas, C. B. Poitras, and M. Lipson, “Silicon nanostructure cloak operating at optical frequencies,” Nat. Photonics **3**, 461–463 (2009). [CrossRef]

**18. **T. Zentgraf, J. Valentine, N. Tapia, J. Li, and X. Zhang, “An optical “Janus” device for integrated photonics,” Adv. Mater. **22**, 2561–2564 (2010). [CrossRef] [PubMed]

**19. **K. K. Y. Lee, Y. Avniel, and S. G. Johnson, “Design strategies and rigorous conditions for single-polarization single-mode waveguides,” Opt. Express **16**, 15170–15184 (2008). [CrossRef] [PubMed]

**20. **R. Ulrich and M. Tacke, “Submillimeter waveguiding on periodic metal structure,” Appl. Phys. Lett. **22**, 251–253 (1973). [CrossRef]

**21. **R. D. Meade, A. Devenyi, J. Joannopoulos, O. Alerhand, D. Smith, and K. Kash, “Novel applications of photonic band gap materials: Low-loss bends and high Q cavities,” J. Appl. Phys. **75**, 4753–4755 (1994). [CrossRef]

**22. **S. Fan, P. R. Villeneuve, J. Joannopoulos, and E. Schubert, “High extraction efficiency of spontaneous emission from slabs of photonic crystals,” Phys. Rev. Lett. **78**, 3294–3297 (1997). [CrossRef]

**23. **S. G. Johnson, S. Fan, P. R. Villeneuve, J. D. Joannopoulos, and L. A. Kolodziejski, “Guided modes in photonic crystal slabs,” Phys. Rev. B **60**, 5751 (1999). [CrossRef]

**24. **M. Qiu, “Effective index method for heterostructure-slab-waveguide-based two-dimensional photonic crystals,” Appl. Phys. Lett. **81**, 1163 (2002). [CrossRef]

**25. **J. D. Joannopoulos, S. G. Johnson, J. N. Winn, and R. D. Meade, *Photonic Crystals: Molding the Flow of Light*, (2nd ed.) (Princeton U. P., 2008).

**26. **J. Witzens, M. Loncar, and A. Scherer, “Self-collimation in planar photonic crystals,” IEEE J. Sel. Top. Quantum Electron. **8**, 1246–1257 (2002). [CrossRef]

**27. **M. Ahmadlou, M. Kamarei, and M. H. Sheikhi, “Negative refraction and focusing analysis in a left-handed material slab and realization with a 3D photonic crystal structure,” J. Opt. A, Pure Appl. Opt. **8**, 199 (2006). [CrossRef]

**28. **J. Zhang, L. Liu, Y. Luo, S. Zhang, and N. A. Mortensen, “Homogeneous optical cloak constructed with uniform layered structures,” Opt. Express **19**, 8625–8631 (2011). [CrossRef] [PubMed]

**29. **X. Chen, T. M. Grzegorczyk, B. I. Wu, J. Pacheco Jr, and J. A. Kong, “Robust method to retrieve the constitutive effective parameters of metamaterials,” Phys. Rev. E **70**, 016608 (2004). [CrossRef]

**30. **M. Hammer and O. V. Ivanova, “Effective index approximations of photonic crystal slabs: a 2-to-1-D assessment,” Opt. Quantum Electron. **41**, 267–283 (2009). [CrossRef]

**31. **S. M. Rytov, “Electromagnetic properties of a finely stratified medium,” Sov. Phys. JETP **2**, 466–475 (1956).

**32. **R. Bräuer and O. Bryngdahl, “Design of antireflection gratings with approximate and rigorous methods,” Appl. Opt. **33**, 7875–7882 (1994). [CrossRef] [PubMed]

**33. **W. Yu, T. Konishi, T. Hamamoto, H. Toyota, T. Yotsuya, and Y. Ichioka, “Polarization-multiplexed diffractive optical elements fabricated by subwavelength structures,” Appl. Opt. **41**, 96–100 (2002). [CrossRef] [PubMed]

**34. **J. A. Kong, *Electromagnetic Wave Theory* (EMW Publishing, 2008).

**35. **S. Johnson and J. Joannopoulos, “Block-iterative frequency-domain methods for Maxwell’s equations in a planewave basis,” Opt. Express **8**, 173–190 (2001). [CrossRef] [PubMed]

**36. **H. Gao, S. Takahashi, L. Tian, and G. Barbastathis, “Aperiodic subwavelength Lüneburg lens with nonlinear Kerr effect compensation,” Opt. Express **19**, 2257–2265 (2011). [CrossRef] [PubMed]

**37. **A. F. Oskooi, D. Roundy, M. Ibanescu, P. Bermel, J. Joannopoulos, and S. G. Johnson, “MEEP: A flexible free-software package for electromagnetic simulations by the FDTD method,” Comput. Phys. Commun. **181**, 687–702 (2010). [CrossRef]