Comprehensive FDTD modelling of photonic crystal waveguide components

doi:10.1364/OPEX.12.000234

Comprehensive FDTD modelling of photonic crystal waveguide components

A. Lavrinenko, P. Borel, L. Frandsen, M. Thorhauge, A. Harpøth, M. Kristensen, T. Niemi, and H. Chong »View Author Affiliations

Optics Express, Vol. 12, Issue 2, pp. 234-248 (2004)
http://dx.doi.org/10.1364/OPEX.12.000234

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▸ Article Outline
– Abstract
1. Introduction
2. Basic features of the FDTD technique
3. Spatial resolution and comparison with band diagrams
4. Comparison with experimental spectra
5. Summary
– References and links

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Abstract

Planar photonic crystal waveguide structures have been modelled using the finite-difference-time-domain method and perfectly matched layers have been employed as boundary conditions. Comprehensive numerical calculations have been performed and compared to experimentally obtained transmission spectra for various photonic crystal waveguides. It is found that within the experimental fabrication tolerances the calculations correctly predict the measured transmission levels and other major transmission features.

1. Introduction

The concept of photonic crystals (PhCs) originated in the late 1980s [1

S. John, “Strong localization of photons in certain disordered dielectric superlattices,” Phys. Rev. Lett. 58, 2486–2489 (1987). [CrossRef] [PubMed]

, 2

E. Yablonovitch, “Inhibited spontaneous emission in solid-state physics and electronics,” Phys. Rev. Lett. 58, 2059–2062 (1987). [CrossRef] [PubMed]

] and these structures are foreseen to be important building blocks in future optoelectronic communication networks. In the beginning, the PhCs were intended for controlling spontaneous emission in optical semiconductor components by exploiting extraordinary properties of periodic structures [3

V. P. Bykov, Radiation of atom in a resonant environment , (World Scientific, Singapore, 1993).

Unfortunately, the practical realization of PhC structures in optics was strongly hampered by a number of obstacles. In this paper we will focus on some the theoretical aspects. Among these, the lack of fast and reliable 3D numerical tools, which are able to cope with fully vectorial Maxwell equations, was a major limitation. The global problem of known numerical recipes was their unstable behavior in a system that includes regions with large difference in their dielectric constant. Needless to say, the requirements for modelling the PhCs are therefore based on the stability properties of the numerical techniques, when handling such abrupt discontinues in the inhomogeneous space function ε(r). One way of overcoming the discontinuities is to increase the spatial resolution of the system, e.g. to increase the number of grid points associated with the characteristic length of the structure. The characteristic length of the PhC is the lattice constant L of the periodical pattern. However, increasing the spatial resolution heavily increases the complexity of the computation as the needed computation resources for most of the methods well known in physics and applied in early era of the PhC modelling scaled nonlinearly with the growing size of the system.

In band diagram calculations of perfect PhCs there is no need to simulate the complete system. It is sufficient to exploit the translation symmetry of the PhC. Thus, only a unit cell of lattice structure must be simulated. When, in turn, the concept of the PhC waveguide (PhCW) appeared, it led to the supercell approach, which could be applied in the computation of planar PhCW structures by choosing the supercell correctly and avoiding any coupling between neighboring supercells. However, full 3D simulations of transmission and reflection were still beyond the range of the existing techniques.

Fortunately, researchers turned to the finite-difference time-domain (FDTD) scheme, known in electromagnetics [4

A. Taflove and S. C. Hagness, Computational electrodynamics: The finite-difference time-domain method , (Artech House, Boston, 2000).

]. Attempts to apply this scheme in the modelling of PhCs were rather successful. Meanwhile, special absorbing boundary conditions, so called perfectly matched layers (PMLs), had been developed that very effectively terminate numerical volumes in 2D and 3D leading to only very small back reflections. The FDTD method implemented with PMLs has recently been widely accepted as a very powerful computational technique in the modelling of PhCs. The complexity of the FDTD method scales only linearly with time and space. Thus, the FDTD scheme is favored compared to most other numerical methods for PhC simulations. However, the FDTD scheme is very demanding in terms of memory and speed of the available computer hardware when applied to practical 3D problems such as analysis of transmission spectra of PhCW in layered structures with 2D patterning. The method does not take full advantage of the periodicity, unlike what is the case in most band diagram calculations. The use of symmetry conditions may only reduce the required memory resources by a factor of four for straight PhCWs. Other passive system elements, such as Y-splitters, zigzags-bends, and vertical couplers have even less symmetry.

The application of FDTD codes to various problems in PhCW design has recently been demonstrated in Refs. [5

S. Fan, “Sharp asymmetric line shapes in side-coupled waveguide-cavity systems,” Appl. Phys. Lett. 80, 908–910 (2002). [CrossRef]

–17

R. Ferrini, D. Leuenberger, M. Mulot, M. Qiu, J. Moosburger, M. Kamp, A. Forchel, S. Anand, and R. Houdré, “Optical study of two-dimensional InP-based photonic crystals by internal light source technique,” IEEE J. Quantum Electron. 38, 786–799 (2002). [CrossRef]

]. Some of the papers [5

S. Fan, “Sharp asymmetric line shapes in side-coupled waveguide-cavity systems,” Appl. Phys. Lett. 80, 908–910 (2002). [CrossRef]

, 6

Y. Sugimoto et al., “Fabrication and characterization of different types of two-dimensional AlGaAs photonic crystal slabs,” J. Appl. Phys. 91, 922–929 (2002). [CrossRef]

, 10

T. Ochiai and K. Sakoda, “Dispersion relation and optical transmittance of a hexagonal photonic crystal slab,” Phys. Rev. B 63, 125107–125113 (2001). [CrossRef]

–12

A. Chutinan and S. Noda, “Waveguide and waveguide bends in two-dimensional photonic crystal slabs,” Phys. Rev. B 62, 4488–4492 (2000). [CrossRef]

, 15

Y. Sugimoto, N. Ikeda, N. Carlsson, K. Asakawa, N. Kawai, and K. Inoue, “AlGaAs-based two-dimensional photonic crystal slab with defect waveguides for planar lightwave circuit applications,” IEEE J. Quantum Electron. 38, 760–769 (2002). [CrossRef]

] address the modelling of transmission spectra in 3D that is essential for studying the features of realistic PhCWs. This applies in particular to the losses of the PhCW modes [9

M. Agio and C. M. Soukoulis, “Ministop bands in single-defect photonic crystal waveguides,” Phys. Rev. E 64, 055603–055606 (2001). [CrossRef]

], which do not appear in 2D calculations. A defect mode in the band gap of a 2D photonic crystal propagates without loss. However, propagation of the defect modes in a 3D system requires basic restrictions of total-internal-reflection to be fulfilled to avoid out-of-plane propagation.

Most of the existing FDTD codes are able to produce qualitatively correct transmission spectra when compared to experimental data. However, frequency discrepancies around 5–10 % or more are often observed, and empirical parameters are in some cases introduced to get better agreement. In this paper we report comprehensive FDTD calculations employing newly developed PML boundary conditions. Analytical formulas for the PMLs are used in the calculations. Special care is taken in the border regions where two or three PMLs overlap. An advantageous consequence of this analytical approach is that it only is necessary to update the E and H fields during the calculations. In addition, a simple spatial representation is utilized allowing the fields in the PMLs and the main region, respectively, to be treated similarly in the calculation cycles. Thereby, the same internal organization of the calculations is ensured everywhere in the modelled structure. We find that our FDTD code produces quantitatively accurate results both regarding the transmission level and spectral features—in all investigated cases frequency shifts below 1–2 % are obtained when comparing numerical data with experimental ones. The paper is organized as follows: First, the basic features of the FDTD method and the PML boundary conditions are presented. Next, the spatial resolution is discussed, and to gain further insight calculated transmission spectra are compared with band-diagrams. Furthermore, the calculated spectra are compared to experimental ones obtained from planar PhCWs realized in silicon-on-insulator material. Finally, in the appendix, a detailed treatment is given of the PMLs.

2. Basic features of the FDTD technique

We use the ONYX-2 version of the FDTD algorithm developed by A. Ward and J. Pendry [18

A. J. Ward and J. B. Pendry, “A program for calculating photonic band structures, Green’s functions and transmission/reflection coefficients using a non-orthogonal FDTD method,” Comput. Phys. Commun. 128, 590–621 (2000). [CrossRef]

] as the basic FORTRAN code. A main characteristic property of the original code is the coinciding space frames for electric and magnetic fields obtained from forward and backward finite difference schemes, respectively, thereby approximating the spatial derivatives. These finite differences are first order approximations to the spatial derivatives and might therefore cause some spurious results. Therefore, the numerical spectra should undergo a careful treatment.

The FDTD algorithm was implemented for an arbitrary system of coordinates in Ref. [18

]. It has been shown that the discrete version of Maxwell equations in an arbitrary grid is given by [19

A. J. Ward and J. B. Pendry, “Refraction and geometry in Maxwell’s equation,” J. Mod. Opt. 43, 773–793 (1996). [CrossRef]

]

Δ_{t}^{+} E (r, t) = ε {(r)}^{- 1} \nabla_{q}^{-} \times H' (r, t), Δ_{t}^{-} H' (r, t) = - Q_{H} μ {(r)}^{- 1} \nabla_{q}^{+} \times E (r, t),

(1)

where QH is a parameter related to the renormalized magnetic field H′, Δ+ _t E=[E(r, t +∂t)-E(r, t)]/∂, and ∇± _q × is the discrete version of the curl operator with spatial derivative approximations like Δ- _iH′ _j =H′ _j (r, t)-H′_j (r-q_i, t) with q_i grid steps in i direction. Similarly, an expression for the second Maxwell’s equation may be given.

In the general case ε(r)^-1 and µ(r)^-1 are inverse tensors of the redefined dielectric permittivity and the magnetic permeability. A useful way of applying the FDTD technique is to utilize a rectangular grid, which may be obtained by expanding a cubic grid in one or two dimensions

ε_{ij} = ε \frac{q_{x} q_{y} q_{z}}{q_{i} q_{j} q_{0}}, μ_{ij} = μ \frac{q_{x} q_{y} q_{z}}{q_{i} q_{j} q_{0}},

(2)

where q_i , i=x, y, z, is the distance between the mesh points in the corresponding directions, and q0 is a characteristic length parameter. Due to the coordinate stretching the dielectric e and magnetic µ constants get tensorial properties. Nevertheless, the usage of coordinate stretching is convenient when treating PhCWs with triangular lattice symmetry. If we for example consider a waveguide in the Γ-K direction (along the x-axis) and with the y-axis in the lattice plane we obtain the following constraint: q_x =q_z =q0=qy/√3. It should be noted that the utilized grids in all cases are strictly orthogonal.

The code also applies to media with loss or gain. However, here we consider only transparent dielectrics, i.e., where the dielectric and magnetic constants are real. In the calculations, the fields are only stored as a function of time for mesh points in detector plates placed directly in the waveguide channel. We avoid allocation of memory for information that is not necessary for a reflection-transmission analysis. At the initial moment the spatial distribution of the electric and the magnetic field describes the incident field [14

M. Qiu and S. He, “Numerical method for computing defect modes in two-dimensional photonic crystals with dielectric or metallic inclusions,” Phys. Rev. B 61, 12871–12876 (2000). [CrossRef]

,18

]. The fields may be designed to excite modes with specific parity, i.e. odd or even. Even if the initial field distribution has non-zero divergence, which corresponds to the existence of a source, the evolution of fields in time keeps the divergence in the whole space constant. This is the clear evidence that the evolving fields are of wave-like nature and are governed by Maxwell equations limited only by unavoidable numerical errors.

The elaboration of the ONYX-2 code for 2D and 3D PhCW problems has required basic modifications of the boundary conditions implemented in the original version [18

]. We have developed a reliable 3D FDTD code by a specific application of absorbing boundary conditions. For reflection-free truncating of the computational space we use uniaxial PMLs, based on considerations by S. Gedney [20]. The advantages of these PMLs over the traditional PMLs introduced by J.P. Berrenger are a more straight procedure for their implementation without splitting of every field component into two parts and saving of memory. The twofold and three-fold intersections of the uniaxial absorbing layers have to be treated with special care. The detailed procedure of the construction of the PMLs is given in the following.

Generally, a PML possess proportional tensors of dielectric and magnetic constants

\tilde{ε} = ε \tilde{Λ}, \tilde{μ} = μ \tilde{Λ},

(3)

where the tensor

\tilde{Λ}

in principal, rectangular coordinates has the form [20

S. D. Gedney, “An anisotropic perfectly matched layer - absorbing medium for the truncation of FDTD lattices,” IEEE Trans. Ant. Prop. 44, 1630–1639 (1996). [CrossRef]

, 21

F. L. Teixeira and W. C. Chew, “On causality and dynamic stability of perfectly matched layers for FDTD simulations,” IEEE Trans. Microw. Theory Technol. 47, 775–785 (1999). [CrossRef]

]

\tilde{Λ} = (\begin{matrix} \frac{s_{y} s_{z}}{s_{x}} & 0 & 0 \\ 0 & \frac{s_{x} s_{z}}{s_{y}} & 0 \\ 0 & 0 & \frac{s_{x} s_{y}}{s_{z}} \end{matrix}),

(4)

The parameters σζ(ζ)≥0 and they usually have the form of a power function σ(ζ)=σ _max(ζ/d) ⁿ , where d is the total thickness of a layer, and n=2,3,4. This form has been proven to provide reflectionless absorption of guided modes. We set the parameters aζ(ζ)=1, however, in order to achieve enhanced absorption, one may set aζ(ζ)>1. The matrix

\tilde{Λ}

describes a biaxial crystal and includes absorption.

\tilde{Λ}

can be represented by a triple matrix product where each matrix is responsible for the expansion along one of the coordinates

\tilde{Λ} (r, ω) = {\tilde{Λ}}_{x} (x, ω) {\tilde{Λ}}_{y} (y, ω) {\tilde{Λ}}_{z} (z, ω),

(6)

where

{\tilde{Λ}}_{x} = (\begin{matrix} \frac{1}{s_{x}} & 0 & 0 \\ 0 & s_{x} & 0 \\ 0 & 0 & s_{x} \end{matrix})

(7)

and similarly for the two other matrices. Tensors

\tilde{Λ}

_ζ (ζ,ω) describe the properties of 1D PML at the faces of the numerical space. Contraction of any two different tensors

\tilde{Λ}

ζ(ζ,ω) gives us 2D PML at the edges of the computational zone. The full matrix

\tilde{Λ}

in Eq. (6) is responsible for the zone corners, where all three 1D PMLs intersect each other.

If we follow the well known approach that Maxwell’s equations in crystals correspond to Maxwell’s equations in isotropic media, but in stretched coordinates [22

W. C. Chew and W. H. Weedon, “A 3-D perfectly matched medium from modified Maxwell’s equations with stretched coordinates,” Microw. Opt. Technol. Lett. 7, 599–604 (1994). [CrossRef]

], the parameters s _ζ (ζ) are nothing else than analytical expansions of real coordinates in the complex plane. The expressions for dielectric and magnetic constants in expanded coordinates are given in Ref. [19

A. J. Ward and J. B. Pendry, “Refraction and geometry in Maxwell’s equation,” J. Mod. Opt. 43, 773–793 (1996). [CrossRef]

]. Exploiting the idea revealed in Refs. [18

, 23

P. G. Petropoulos, L. Zhao, and A. C. Cangellaris, “A reflectionless sponge layer absorbing boundary condition for the solution of Maxwell’s equations with high-order staggered finite difference schemes,” J. Comput. Phys. 139, 184–208 (1998). [CrossRef]

] we can show that the numerical algorithm for the implementation of 2D PML at the edge, corresponding to the k coordinate, is as follows (for derivation, see Appendix):

E_{i} (t + \partial t) = \frac{1}{1 + σ_{j} \partial t} {E_{i} (t) + \frac{1}{ε_{ii}} {[\nabla_{q} \times H' (t)]}_{i} + \frac{σ_{i} \partial_{t}}{ε_{ii}} \sum_{n = 0}^{\infty} {[\nabla_{q} \times H' (t - n \partial t)]}_{i}}

E_{j} (t + \partial t) = \frac{1}{1 + σ_{i} \partial t} {E_{j} (t) + \frac{1}{ε_{jj}} {[\nabla_{q} \times H' (t)]}_{j} + \frac{σ_{j} \partial_{t}}{ε_{jj}} \sum_{n = 0}^{\infty} {[\nabla_{q} \times H' (t - n \partial t)]}_{j}}

E_{k} (t + \partial t) = \frac{E_{k} (t) - σ_{i} σ_{j} \partial t^{2} \sum_{n = 0}^{\infty} E_{k} (t - n \partial t) + {(\nabla \times H' (t))}_{k} ⁄ ε_{kk}}{1 + (σ_{i} + σ_{j}) \partial t + σ_{i} σ_{j} \partial t^{2}}

H_{i}^{'} (t) = \frac{1}{1 + σ_{j} \partial t} \times

{H_{i}^{'} (t - \partial t) - \frac{Q_{H}}{μ_{ii}} {[\nabla_{q} \times E (t)]}_{i} - \frac{σ_{i} \partial t}{μ_{ii}} Q_{H} \sum_{n = 0}^{\infty} {[\nabla_{q} \times E (t - n \partial t)]}_{i}}

H_{j}^{'} (t) = \frac{1}{1 + σ_{i} \partial t} \times

{H_{j}^{'} (t - \partial t) - \frac{Q_{H}}{μ_{jj}} {[\nabla_{q} \times E (t)]}_{j} - \frac{σ_{j} \partial t}{μ_{jj}} Q_{H} \sum_{n = 0}^{\infty} {[\nabla_{q} \times E (t - n \partial t)]}_{j}}

H_{k}^{'} (t) = \frac{H_{k}^{'} (t - \partial t) - σ_{i} σ_{j} \partial t^{2} \sum_{n = 0}^{\infty} H_{k}^{'} (t - \partial t - n \partial t) - Q_{H} {(\nabla \times E (t))}_{k} ⁄ μ_{kk}}{1 + (σ_{i} + σ_{j}) \partial t + σ_{i} σ_{j} \partial t^{2}} .

(8)

Here, electric and magnetic field components are redefined according to the scheme presented in Ref. [18

]. The same ideas can be straightforwardly applied for the implementation of 3D PML.

3. Spatial resolution and comparison with band diagrams

We have done an extensive variety of different 2D and 3D calculations of various components including straight PhCWs of different lengths, various PhCW bend geometries, and other PhC structures utilizing our improved FDTD code. The outcome of the calculations is the transmission and reflection spectra for these PhC structures. The calculations were carried out by utilizing a straight PhCW as the basic element. We use W1 PhCWs, i.e., waveguides where the defect is formed by removing one row of holes in the Γ-K direction. The typical size of the memory allocated for 2D calculations is about 100 Mb depending on the number of time steps. Usually there were 2¹³ steps in time, but the number of time steps was in some cases increased to 2¹⁴–2¹⁶ to obtain better resolution. For 3D calculations with reasonable choice of width, thickness and length, the memory requirements increased to 800–900 Mb. The CPU time is strongly dependent on processor frequency and optimization features provided by the FORTRAN compiler.

3.1. Spatial resolution

The spatial resolution of the simulated structure is given as the number of mesh points used for the discretization of space within one lattice constant Λ. The resolution is one of the major parameters that determines the needed computation time and the consumption of memory resources as well as the accuracy of the computation. The photonic crystal structure is embedded in a substrate (silicon) with ε=12. The holes have a radius of 0.375Λ and the inner side is coated with a layer of low refractive index material (silica). The thickness of the coating is 0.125Λ and its refractive index is 1.45. In the vertical direction the 3D structures consist of 3–4 layers of dielectric material placed on a substrate or suspended in air. In order to investigate the effect of the spatial resolution on the results of the simulations we performed similar calculations increasing the spatial resolution from 16 to 32 and even 64 mesh points per period Λ. Computed transmission spectra for TE polarized light in 2D for a straight 15Λ long PhCW are given in Fig. 1(a). It is evident that the Λ/64 mesh structure is more accurate, when comparing it with 2D-calculations of a 10Λ long PhCW performed by Agio in Ref. [9

M. Agio and C. M. Soukoulis, “Ministop bands in single-defect photonic crystal waveguides,” Phys. Rev. E 64, 055603–055606 (2001). [CrossRef]

]. However, the spectra are in general quite similar except the dip at frequency Λ/λ=0.26. This frequency corresponds to the cross-section point of an even and an odd mode as shown in Fig. 2. The dip can be explained by a broken symmetry of the simulated structure when first-order finite differences are applied. Therefore, numerically induced interactions between even and odd modes are unavoidable and an artificial anti-crossing effect between the even and the odd mode leads to the artificial mini stop-zone and hence, the dip in the transmission spectrum. Increasing the spatial resolution reduces the numerical coupling and the dip eventually disappears. By increasing the resolution from Λ/16 the computing time increases by a factor of 4 and 16 for resolutions of Λ/32 and Λ/64, respectively, in a 2D system. Calculated 3D transmission spectra for the straight W1 PhCW with 16 and 32 mesh points per Λ are presented in Fig. 1(b). Again, we see a very good resemblance between the two spectra except for the artificial dip corresponding to the odd-even mode intersection at Λ/λ=0.31. Therefore, we conclude that performing the FDTD calculations with a spatial resolution of 16 mesh points per Λ is sufficient in order to reveal the main features of the transmission through a straight PhCW. Specific features may have to be analyzed using a higher number of mesh points.

Fig. 1. Transmission spectra for a PhCW calculated for (a) three different spatial resolutions in 2D (b) two different spatial resolutions in 3D.

3.2. Comparison of transmission spectra and band diagrams

In this section we make direct comparisons between 2D transmission spectra and corresponding band diagrams for TE polarized light. Figure 2 shows the band diagrams (left) calculated by using plane wave expansion theory (PWE) [24

S. G. Johnson and J. D. Joannopoulos, “Block-iterative frequency-domain methods for Maxwell’s equations in a planewave basis,” Opt. Express 8, 173–190 (2001), http://www.opticsexpress.org/abstract.cfm?URI=OPEX-8-3-173 [CrossRef] [PubMed]

] and the related transmission spectra (right) simulated by using FDTD (both in 2D) for a W1 PhCW. The correlation between the band diagram and the transmission spectrum is excellent, it is seen that all the major features in the band diagram are directly relatable to features in the transmission spectrum. The largest dip in the transmission spectrum is observed at Λ/λ=0.22-0.23, and it is due to the complete absence of modes in this frequency region. High transmission is observed for the index guided mode below Λ/λ=0.17 and Λ/λ=0.18-0.19 and for the even photonic band gap mode Λ/λ=0.22-0.31. At Λ/λ=0.26 the dip in the transmission curve is due to the spurious mini stop-zone caused by the artificial anti-crossing effect between the even and the odd mode as discussed in Section 3.1.

4. Comparison with experimental spectra

To confirm the predictions of our FDTD code a number of planar PhCWs have been fabricated in silicon-on-insulator material. First, the experimental fabrication procedure is discussed. Thereafter, measured transmission spectra are compared to the calculated ones.

Fig. 2. 2D Band diagram (left) shown for modes of different parities in a W1 PhCW. Even guided modes are shown in red, odd modes in blue, and slab modes in black. Transmission spectrum (right) shown for excitation with even modes.

4.1. Fabrication of SOI PhCWs

The PhCs are fabricated as triangular arrangements of air holes in a SiO₂/Si/SiO₂ trilayer film. The thicknesses of the layers are 50 nm/300 nm/1 µm, respectively. E-beam lithography is used to define the PhC pattern in an e-beam resist, which is used as mask in a reactive ion etch (RIE) of the top silicon layer on the initial silicon-on-insulator wafer. The perforated top silicon layer is used as a mask in a subsequent RIE of silica to make the PhC pattern penetrate ~100 nm down into the underlying silica layer. The reason for not letting the PhC holes penetrate deep into the silica layer is the low selectivity in the RIE between silicon and silica. Finally, in order to increase the vertical symmetry of the PhC structure and to smoothen out any surface roughness, a thin oxide layer (~50 nm) is grown on top of the structure by thermal oxidation. The final diameter of the PhC holes is D _glass=0.76Λ, where Λ=428 nm is the lattice pitch. Figure 3 shows representative scanning electron micrographs of (a) a fabricated 10 µm straight W1 PhCW and (b) a PhCW containing two 60° bends.

The characterization setup used to measure the transmission spectra of the fabricated waveguides has been described in detail elsewhere [25

P. I. Borel et al., “Efficient propagation of TM polarized light in photonic crystal components exhibiting band gaps for TE polarized light,” Opt. Express 11, 1757–1762 (2003), http://www.opticsexpress.org/abstract.cfm?URI=OPEX-11-15-1757 [CrossRef] [PubMed]

4.2. Estimation of propagation losses

Next, we will compare transmission spectra calculated using our 3D FDTD code to experimental transmission spectra obtained from measurements. It is well known that the main loss in a planar PhCW is caused by out-of-plane scattering of energy. This means that coupling of PhCW modes to radiative modes, which are capable of propagating in the ambient medium, strongly increases the propagation loss of modes in the PBG. Therefore, we expect that 2D transmission calculations do not provide such characteristics of the PhCW (see e.g. Ref. [9

M. Agio and C. M. Soukoulis, “Ministop bands in single-defect photonic crystal waveguides,” Phys. Rev. E 64, 055603–055606 (2001). [CrossRef]

]). It has previously been attempted to calculate the transmission loss due to the out-of-plane scattering in 3D PhCWs using 2D simulations by making the material in the holes absorptive. In this way, it is possible to obtain 2D transmission spectra, which are in agreement with experimental spectra [26

H. Benisty et al., “Radiation losses of waveguide-based two-dimensional photonic crystals: Positive role of the substrate,” Appl. Phys. Lett. 76, 532–534 (2000). [CrossRef]

], and use these to estimate the waveguide losses. However, the method represents a crude approximation and the results cannot be compared directly to experiments. A logical conclusion is that only full 3D transmission calculations are adequate for numerical estimations of genuine PhCW transmission. For the modelling of the propagation losses in the PhCW we used the experimental parameters of planar silicon-on-insulator PhCWs. Hence, the PhCW is defined as a line defect in the Γ-K direction of a triangular lattice of holes. The physical parameters such as hole diameters and dimensions of vertical structure were chosen to match the experimental ones as closely as possible. 3D FDTD calculations have shown that 5 rows of holes on both sides of the waveguide line defect are enough to pin the light to the core. Both in the calculations and the experiment we utilized 10 rows of holes on each side. In the calculations the length of the waveguides was varied from 10Λ to 60Λ. Figure 4(a) shows 3 representative calculations of the 3D transmission through PhCWs with different lengths for TE polarized light. Figure 4(b) shows the measured and calculated transmission spectra for the 10 µm (23Λ) straight W1 PhCW displayed in Fig. 3(a) for TE polarized light. The measured spectrum has been normalized to the transmission spectrum for a ridge waveguide located on the same sample. From the figure it is evident that the 3D FDTD calculations successfully explain all essential features of the spectrum as well as the actual transmission level. The position of the sharp cut-off around 1540 nm is in excellent agreement with previous band gap calculations [28

T. Søndergaard, J. Arentoft, and M. Kristensen, “Theoretical analysis of finite-height semiconductor-on-insulator based planar photonic crystal waveguides,” J. Lightwave Technol. 20, 1619–1626 (2002). [CrossRef]

]. The small frequency shift (approximately 1–2%) between the experimental and simulated spectra is due to uncertainties of the experimental parameters and the limited grid resolution of the 3D FDTD calculations. For wavelengths longer than ~1540 nm the measured transmission appears to be less suppressed than the calculated one. This is due to the fact that it experimentally not is possible to completely extinguish the TM polarization. In Ref. [25

] it was found that TM polarized light propagates with very low loss in straight PhCWs in this wavelength range. Hence, the measured transmission will unavoidably include a small part of TM polarized light, and this small TM contribution plays a rather significant role at the longer wavelengths, where there are no guided TE polarized modes in the PhCW. The calculations, however, are performed utilizing a purely TE polarized light source.

Fig. 3. Scanning electron micrographs of (a) a straight PhCW of length 10 µm, and (b) a PhCW containing two modified 60° bends (details shown in zoom), which are separated by a 20Λ long straight PhCW.

Fig. 4. (a) 3D FDTD transmission spectra for different lengths of PhCW. (b) The measured (gray) and calculated (dashed black) transmission spectra for a 10 µm PhCW.

In order to experimentally find the propagation loss in straight PhCWs we have fabricated and characterized seven straight PhCWs of different lengths between 10 µm–150 µm. For a given wavelength the propagation loss can be extracted by finding the slope of the best linear fit, when plotting the transmission on a logarithmic scale as function of the PhCW length. Similarly, the calculated propagation loss is found from the transmission through PhCWs with lengths 10–60Λ. Figure 5 shows the measured and calculated propagation loss for TE polarized light. Again excellent agreement is seen between experiment and simulation.

Fig. 5. The measured (gray) and calculated (dashed black) propagation losses for the TE polarization.

Numerically, we have also investigated the dependence of the transmission on the vertical structure. By changing the thickness of the air and the silica above and under the core layer in the computations and keeping other parameters fixed we observed the following tendency: For a thickness of the complete vertical structure at 500 nm the lowest propagation loss was found to be 108 dB/mm. When the thickness was increased to 1100 nm propagation losses like the ones displayed in Fig. 5 were obtained. Further increase of the cladding thickness did not improve the transmission. These calculations show that it is important to have enough vertical space for leaky (i.e. radiating) modes to travel along the waveguide, since these modes otherwise would be cut immediately by the PMLs.

Fig. 6. Measured (gray) and calculated (dashed black) bend loss in two consecutive 60° bends for the TE polarization.

4.3. Sixty degree bends

It is an essential property for all integrated photonic circuits to be able to route the light around sharp corners. The natural bend in a PhC defined in a triangular lattice is the 60° bend. Figure 3(b) shows a fabricated PhCW having two consecutive 60° bends separated by an intermediate PhCW with length 20Λ. Each bend has been modified by displacing one hole in the bend. The recorded transmission spectrum for TE polarized light has been normalized to the transmission spectrum for a straight PhCW of same length. The normalized spectrum, which now expresses the total bend loss for the two 60° bends in the PhCW, is shown in Fig. 6. The figure also shows the calculated bend loss for a PhCW containing two similar 60° bends separated by 20Λ. It is seen that the 3D FDTD simulations successfully explain the observed bend losses and the spectral features. Losses as small as 1.6 dB per bend are observed in the shown wavelength region. The oscillations observed in the spectrum have conclusively been identified as Fabry-Perot resonances by recording experimental spectra for PhCWs having different lengths (20–40Λ) of the intermediate straight PhCW connecting the two bends. The Fabry-Perot cavity oscillations in the measured and simulated spectra are found to be in very good agreement. The frequency shift between the measured and calculated local maxima and minima is found to be around 1 %. Further experiments have shown that the bend geometry shown in Fig. 3(b) has improved the transmission per bend by 4–5 dB compared to unmodified sharp 60° bends in the displayed wavelength region in Fig. 6.

4.4. Other structures, geometries and polarizations

Several other comparisons between experimental spectra and numerical spectra obtained using the FDTD code have been performed. A few of these results have already been reported in the literature. For example, for the straight PhCWs shown in Fig. 3(a) we have experimentally demonstrated a broad wavelength span with high transmission for the TM polarization and propagation losses as low as 2.5 dB/mm have been measured [25

]. These findings have successfully been confirmed by 3D FDTD calculations. Furthermore, directional couplers with coupling losses just above 1 dB have been fabricated in SOI material [25

, 30

M. Thorhauge, L. H. Frandsen, and P. I. Borel, “Efficient Photonic Crystal Directional Couplers,” Opt. Lett. 28, 1525–1527 (2003). [CrossRef] [PubMed]

]. Again the measured transmission levels and spectral features are in excellent agreement with the 3D FDTD calculations both for the TE and TM polarizations.

Recently, McNab and Vlasov [31

S. J. McMab and Y. A. Vlasov, “SOI 2D photonic crystals for microphotonic integrated circuits,” Holey fibers and photonic crystals, (Digest of IEEE-LEOS Summer Topical Meetings, Vancouver, 2003) pp. 79–80.

] have experimentally obtained propagation losses at 1.7 dB/mm for TE polarized light in planar W1 PhCWs realized in a silicon-in-air membrane. We have performed 3D FDTD calculations that quantitatively confirm their reported transmission level and spectral features. The reason for the lower losses for TE polarized light in this case compared to the losses reported in Fig. 5 is that for the silicon-membrane waveguides there is a large section of a TE polarized photonic band gap guided mode below the light line. For the silicon-on-insulator waveguides this mode is mostly located above the light line, whereby it becomes leaky and has out-of-plane scattering losses.

5. Summary

In this paper details on 2D and 3D finite-difference-time-domain calculations have been reported for planar photonic crystal waveguide structures, where perfectly matched layers have been employed as boundary conditions. For the calculated transmission spectra it was found that a spatial resolution at Λ/16 was sufficient to correctly reproduce most spectral features and that an even better result was obtained when the resolution was increased to Λ/32. Calculated spectra for various photonic crystal structures have been compared to experimental spectra. In all cases an excellent agreement has been found both regarding the transmission level and the spectral features. Hence, we have developed a finite-difference-time-domain code that gives quantitatively correct results without the use of any empirical parameters.

This work was supported in part by the European IST project PICCO.

Appendices

A. Appendix

In Section 2 it was discussed that the discrete version of Maxwell’s equations in an arbitrary coordinate system may be written as shown in Eq. 1. In the most important case of a rectangular grid expressions for ε_ij and µ_ij were given in Eq. 2. The coordinate stretching in a rectangular grid results in tensorial properties for the dielectric and magnetic constants. In the PML regions these properties will be superimposed by anisotropic properties of the PML itself. For example, in a 1D PML orthogonal to the z axis, we have

{\tilde{ε}}_{xx} = ε_{xx} (1 + \frac{i σ_{z}}{ω^{-}}), {\tilde{ε}}_{yy} = ε_{yy} (1 + \frac{i σ_{z}}{ω^{-}}), {\tilde{ε}}_{zz} = ε_{zz} {(1 + \frac{i σ_{z}}{ω^{-}})}^{- 1},

(9)

where the components ε_ij are defined by Eq. (2), σ _z =σ(z), and

ω^{-} = \frac{1 - \exp (i ω \partial t)}{- i \partial t}

is a discretized frequency [18

]. Using Eq. (1) for the x component of the electric field we obtain

E_{x} (t + \partial t) - E_{x} (t) = {({\tilde{ε}}^{- 1})}_{xx} {[\nabla_{q} \times H' (t)]}_{x} = \frac{1}{ε_{xx}} {(1 + \frac{i σ_{z}}{ω^{-}})}^{- 1} {[\nabla_{q} \times H' (t)]}_{x} .

(10)

The x-component of the curl operator may be approximated by [18

]

{[\nabla_{q} \times H']}_{x} = - i \partial t ε_{xx} ω^{+} (1 + \frac{i σ_{z}}{ω^{-}}) E_{x}

(11)

with

ω^{+} = \frac{\exp (- i ω \partial t) - 1}{- i \partial t}

. Straightforward derivations give us the result [18

]

E_{x} (t + \partial t) = E_{x} (t) + \frac{1}{ε_{xx}} {(1 + \frac{i σ_{z}}{ω^{-}})}^{- 1} {[\nabla_{q} \times H' (t)]}_{x}

= \frac{1 + σ_{z} \partial t}{1 + σ_{z} \partial t} E_{x} (t) + \frac{1}{ε_{xx}} {(1 + \frac{i σ_{z}}{ω^{-}})}^{- 1} {[\nabla_{q} \times H' (t)]}_{x}

= \frac{1}{1 + σ_{z} \partial t} E_{x} (t) + \frac{σ_{z} \partial t}{1 + σ_{z} \partial t} E_{x} (t) + \frac{1}{ε_{xx}} \frac{ω^{-}}{ω^{-} + i σ_{z}} {[\nabla_{q} \times H' (t)]}_{x}

\frac{1}{1 + σ_{z} \partial t} E_{x} (t) + \frac{{[\nabla_{q} \times H' (t)]}_{x}}{ε_{xx} (1 + σ_{z} \partial t)} \times [\frac{i ω^{-} σ_{z}}{ω^{+} (ω^{-} + i σ_{z})} + \frac{ω^{-} (1 + σ_{z} \partial t)}{ω^{-} + i σ_{z}}]

= \frac{1}{1 + σ_{z} \partial t} (E_{x} (t) + \frac{{[\nabla_{q} \times H' (t)]}_{x}}{ε_{xx}}) .

(12)

The corresponding expression follows for E_y . The z-component is treated differently. From Eq. (1) we obtain

E_{z} (t + \partial t) = E_{z} (t) + \frac{1}{ε_{zz}} (1 + \frac{i σ_{z}}{ω^{-}}) {[\nabla_{q} \times H' (t)]}_{z}

= E_{z} (t) + \frac{1}{ε_{zz}} {[\nabla_{q} \times H' (t)]}_{z} + \frac{i σ_{z}}{ε_{zz}} \cdot \frac{- i \partial t}{1 - e^{i ω \partial t}} {[\nabla_{q} \times H' (t)]}_{z}

= E_{z} (t) + \frac{1}{ε_{zz}} {[\nabla_{q} \times H' (t)]}_{z} + \frac{σ_{z} \partial t}{ε_{zz}} \cdot {\sum_{n = 0}^{\infty} e^{in ω \partial t} [\nabla_{q} \times H' (t)]}_{z}

= E_{z} (t) + \frac{1}{ε_{zz}} {[\nabla_{q} \times H' (t)]}_{z} + \frac{σ_{z} \partial t}{ε_{zz}} \cdot {\sum_{n = 0}^{\infty} [\nabla_{q} \times H' (t - n \partial t)]}_{z} .

(13)

It is seen from Eqs. (12) and (13) that the components of the electromagnetic fields lying in the plane of PML layer are decreasing with the same rate while penetrating deeper inside the layer. The fields in anisotropic absorbing medium propagate as directed by Maxwell equations. During the numerical implementation the infinite series are substituted by finite sums. For the field evolution by the FDTD method this means that the summation will commence at the initial pulse.

The results obtained above were presented byWard and Pendry in Ref. [18

]. They have been included here for convenience. Next we proceed to the 2D PML case. For the x-y edge PML the matrix for the dielectric tensor ε̃ in principal coordinates is given by

\tilde{ε} = (\begin{matrix} ε_{11} \frac{1 + \frac{i σ_{y}}{ω^{-}}}{1 + \frac{i σ_{x}}{ω^{-}}} & 0 & 0 \\ 0 & ε_{22} \frac{1 + \frac{i σ_{x}}{ω^{-}}}{1 + \frac{i σ_{y}}{ω^{-}}} & 0 \\ 0 & 0 & ε_{33} (1 + \frac{i σ_{x}}{ω^{-}}) (1 + \frac{i σ_{y}}{ω^{-}}) \end{matrix}) .

(14)

Instead of expression (10) for the x projection of Maxwell equations (1) we have

E_{x} (t + \partial t) - E_{x} (t) = {({\tilde{ε}}^{- 1})}_{xx} {[\nabla_{q} \times H' (t)]}_{x}

= \frac{1}{ε_{xx}} (1 + \frac{i σ_{x}}{ω^{-}}) {(1 + \frac{i σ_{y}}{ω^{-}})}^{- 1} {[\nabla_{q} \times H' (t)]}_{x} .

(15)

It is seen from Eq. (12) that the factor

(1 + \frac{i σ_{y}}{ω^{-}})

in the denominator corresponds to multiplication of all field components by the factor

\frac{1}{1 + σ_{y} \partial t}

. As seen from Eq. (13) the presence of this factor in the nominator leads to the appearance of the curl summed over all previous time steps. Because these actions are independent we can also write

E_{x} (t + \partial t) = \frac{1}{1 + σ_{y} \partial t} \times

{E_{x} (t) + \frac{1}{ε_{xx}} {[\nabla_{q} \times H' (t)]}_{x} + \frac{σ_{x} \partial t}{ε_{xx}} \cdot \sum_{n = 0}^{\infty} {[\nabla_{q} \times H' (t - n \partial t)]}_{x}}

(16)

A similar expression may be written for the y projection of the vector E. However, for the z-component of E both factors are in the nominator

E_{z} (t + \partial t) - E_{z} (t) = {({\tilde{ε}}^{- 1})}_{zz} {[\nabla_{q} \times H' (t)]}_{z}

= \frac{1}{ε_{zz}} {(1 + \frac{i σ_{x}}{ω^{-}})}^{- 1} {(1 + \frac{i σ_{y}}{ω^{-}})}^{- 1} {[\nabla_{q} \times H' (t)]}_{z} .

(17)

In this case we are not able to make derivations of each bracket independently. So we start from the beginning rearranging the expression to the form

(1 + \frac{i σ_{x}}{ω^{-}}) (1 + \frac{i σ_{y}}{ω^{-}}) (E_{z} (t + \partial t) - E_{2} (t)) =

(1 + \frac{i (σ_{x} + σ_{y})}{ω^{-}} - \frac{σ_{x} σ_{y}}{{(ω^{-})}^{2}}) (E_{z} (t + \partial t) - E_{z} (t)) .

(18)

Taking this expression by parts we obtain

\frac{i (σ_{x} + σ_{y})}{ω^{-}} (E_{z} (t + \partial t) - E_{z} (t)) = i \frac{(σ_{x} + σ_{y}) (- i \partial t)}{1 - e^{i ω σ t}} (E_{z} (t + \partial t) - E_{z} (t))

= (σ_{x} + σ_{y}) \partial t \sum_{k = 0}^{\infty} e^{- ki ω \partial t} (E_{z} (t + \partial t) - E_{z} (t))

= (σ_{x} + σ_{y}) \partial t \times

(\sum_{k = 0}^{\infty} E_{z} (t + \partial t - k \partial t) - \sum_{k = 0}^{\infty} E_{z} (t - k \partial t))

= (σ_{x} + σ_{y}) \partial t E_{z} (t + \partial t);

(19)

\frac{σ_{x} σ_{y}}{{(ω^{-})}^{2}} (E_{z} (t + \partial t) - E_{z} (t)) = \frac{σ_{x} σ_{y}}{ω^{-}} \frac{- i \partial t}{1 - e^{i ω \partial t}} (E_{z} (t + \partial t) - E_{z} (t))

= - i \partial t \frac{σ_{x} σ_{y}}{ω^{-}} E_{z} (t + \partial t)

= \frac{{(- i \partial t)}^{2} σ_{x} σ_{y}}{1 - e^{i ω \partial t}} E_{z} (t + \partial t)

= - \partial t^{2} σ_{x} σ_{y} \sum_{k = 0}^{\infty} E_{z} (t + \partial t - k \partial t)

= - \partial t^{2} σ_{x} σ_{y} (E_{z} (t + \partial t) + \sum_{k = 0}^{\infty} E_{z} (t - k \partial t)) .

(20)

Collecting all parts together give

\frac{1}{ε_{zz}} {[\nabla_{q} \times H' (t)]}_{z} = E_{z} (t + \partial t) - E_{z} (t) + \partial t (σ_{x} + σ_{y}) E_{z} (t + \partial t) +

\partial t^{2} σ_{x} σ_{y} (E_{z} (t + \partial t) + \sum_{k = 0}^{\infty} E_{z} (t - k \partial t)) .

(21)

Finally, the old field components are used to derive the new one

E_{z} (t + \partial t) = \frac{E_{z} (t) - σ_{x} σ_{y} \partial t^{2} \sum_{k = 0}^{\infty} E_{z} (t - k \partial t) + {(\nabla \times H' (t))}_{z} ⁄ ε_{zz}}{1 + (σ_{x} + σ_{y}) \partial t + σ_{x} σ_{y} \partial t^{2}} .

(22)

All other 2D PML’s are treated in a similar way and it is possible to write down the expressions immediately, using the cycling of indices: x→y, y→z, z→x. The same holds true for the derivation of the evolution equation for the magnetic field components.

The corresponding matrix for a 3D PML is

\tilde{ε} = (\begin{matrix} ε_{xx} \frac{(1 + \frac{i σ_{y}}{ω^{-}}) (1 + \frac{i σ_{z}}{ω^{-}})}{1 + \frac{i σ_{x}}{ω^{-}}} & 0 & 0 \\ 0 & ε_{yy} \frac{(1 + \frac{i σ_{x}}{ω^{-}}) (1 + \frac{i σ_{z}}{ω^{-}})}{1 + \frac{i σ_{y}}{ω^{-}}} & 0 \\ 0 & 0 & ε_{zz} \frac{(1 + \frac{i σ_{x}}{ω^{-}}) (1 + \frac{i σ_{y}}{ω^{-}})}{1 + \frac{i σ_{z}}{ω^{-}}} \end{matrix}) .

(23)

It is obvious that the 3D PML described by Eq. (23) has a similar influence on the field components. The derivation of the evolution equations corresponding to Eqs. (13) and (22) is cumbersome, but straightforward.

Finally, we would like to make a remark. Instead of the procedure applied in the derivation of Eq. (22) it is possible to use 2D boundary conditions in the form discussed by Petropoulos and Zhao [23

] e.g., for the z-component of the electric field

ε_{zz} \frac{\partial E_{z}}{\partial t} + ε_{zz} (σ_{x} + σ_{y}) E_{z} + ε_{zz} σ_{x} σ_{y} \int_{0}^{t} {\tilde{E}}_{z} (t') dt' = {(\nabla \times H')}_{z} .

(24)

Taking into account the time positions of the electric and magnetic fields in the FDTD scheme all the features of Eq. (22) are seen from Eq. (24), and it may be used to obtain the same result. The latter expression for the boundary conditions has more physical insight on the transformation of the PML at the crossing zones into time domain. However, our derivation through Eqs. (14)–(22) seems more straightforward from the point of view of direct numerical applications.

References and links

1.	S. John, “Strong localization of photons in certain disordered dielectric superlattices,” Phys. Rev. Lett. 58, 2486–2489 (1987). [CrossRef] [PubMed]
2.	E. Yablonovitch, “Inhibited spontaneous emission in solid-state physics and electronics,” Phys. Rev. Lett. 58, 2059–2062 (1987). [CrossRef] [PubMed]
3.	V. P. Bykov, Radiation of atom in a resonant environment , (World Scientific, Singapore, 1993).
4.	A. Taflove and S. C. Hagness, Computational electrodynamics: The finite-difference time-domain method , (Artech House, Boston, 2000).
5.	S. Fan, “Sharp asymmetric line shapes in side-coupled waveguide-cavity systems,” Appl. Phys. Lett. 80, 908–910 (2002). [CrossRef]
6.	Y. Sugimoto et al., “Fabrication and characterization of different types of two-dimensional AlGaAs photonic crystal slabs,” J. Appl. Phys. 91, 922–929 (2002). [CrossRef]
7.	K. Yamada et al., “Improved line-defect structures for photonic-crystal waveguides with high group velocity,” Opt. Commun. 198, 395–402 (2001). [CrossRef]
8.	M. Loncar et al., “Methods for controlling positions of guided modes of photonic-crystal waveguides,” J. Opt. Soc. Am. B 9, 1362–1368 (2001). [CrossRef]
9.	M. Agio and C. M. Soukoulis, “Ministop bands in single-defect photonic crystal waveguides,” Phys. Rev. E 64, 055603–055606 (2001). [CrossRef]
10.	T. Ochiai and K. Sakoda, “Dispersion relation and optical transmittance of a hexagonal photonic crystal slab,” Phys. Rev. B 63, 125107–125113 (2001). [CrossRef]
11.	E. Chow et al., “Quantitative analysis of bending efficiency in photonic-crystal waveguide bends at λ=1.55 µm wavelengths,” Opt. Lett. 26, 286–288 (2001). [CrossRef]
12.	A. Chutinan and S. Noda, “Waveguide and waveguide bends in two-dimensional photonic crystal slabs,” Phys. Rev. B 62, 4488–4492 (2000). [CrossRef]
13.	A. Adibi et al., “Properties of the slab modes in photonic crystal optical waveguides,” J. Lightwave Technol. 18, 1554–1564 (2000). [CrossRef]
14.	M. Qiu and S. He, “Numerical method for computing defect modes in two-dimensional photonic crystals with dielectric or metallic inclusions,” Phys. Rev. B 61, 12871–12876 (2000). [CrossRef]
15.	Y. Sugimoto, N. Ikeda, N. Carlsson, K. Asakawa, N. Kawai, and K. Inoue, “AlGaAs-based two-dimensional photonic crystal slab with defect waveguides for planar lightwave circuit applications,” IEEE J. Quantum Electron. 38, 760–769 (2002). [CrossRef]
16.	H. Benisty et al., “Models and measurements for the transmission of submicron-width waveguide bends defined in two-dimensional photonic crystals,” IEEE J. Quantum Electron. 38, 770–785 (2002). [CrossRef]
17.	R. Ferrini, D. Leuenberger, M. Mulot, M. Qiu, J. Moosburger, M. Kamp, A. Forchel, S. Anand, and R. Houdré, “Optical study of two-dimensional InP-based photonic crystals by internal light source technique,” IEEE J. Quantum Electron. 38, 786–799 (2002). [CrossRef]
18.	A. J. Ward and J. B. Pendry, “A program for calculating photonic band structures, Green’s functions and transmission/reflection coefficients using a non-orthogonal FDTD method,” Comput. Phys. Commun. 128, 590–621 (2000). [CrossRef]
19.	A. J. Ward and J. B. Pendry, “Refraction and geometry in Maxwell’s equation,” J. Mod. Opt. 43, 773–793 (1996). [CrossRef]
20.	S. D. Gedney, “An anisotropic perfectly matched layer - absorbing medium for the truncation of FDTD lattices,” IEEE Trans. Ant. Prop. 44, 1630–1639 (1996). [CrossRef]
21.	F. L. Teixeira and W. C. Chew, “On causality and dynamic stability of perfectly matched layers for FDTD simulations,” IEEE Trans. Microw. Theory Technol. 47, 775–785 (1999). [CrossRef]
22.	W. C. Chew and W. H. Weedon, “A 3-D perfectly matched medium from modified Maxwell’s equations with stretched coordinates,” Microw. Opt. Technol. Lett. 7, 599–604 (1994). [CrossRef]
23.	P. G. Petropoulos, L. Zhao, and A. C. Cangellaris, “A reflectionless sponge layer absorbing boundary condition for the solution of Maxwell’s equations with high-order staggered finite difference schemes,” J. Comput. Phys. 139, 184–208 (1998). [CrossRef]
24.	S. G. Johnson and J. D. Joannopoulos, “Block-iterative frequency-domain methods for Maxwell’s equations in a planewave basis,” Opt. Express 8, 173–190 (2001), http://www.opticsexpress.org/abstract.cfm?URI=OPEX-8-3-173 [CrossRef] [PubMed]
25.	P. I. Borel et al., “Efficient propagation of TM polarized light in photonic crystal components exhibiting band gaps for TE polarized light,” Opt. Express 11, 1757–1762 (2003), http://www.opticsexpress.org/abstract.cfm?URI=OPEX-11-15-1757 [CrossRef] [PubMed]
26.	H. Benisty et al., “Radiation losses of waveguide-based two-dimensional photonic crystals: Positive role of the substrate,” Appl. Phys. Lett. 76, 532–534 (2000). [CrossRef]
27.	J. D. Joannopoulos, R. D. Meade, and J. N. Winn, Photonic crystals: Molding the flow of light , (Princeton University Press, 1995).
28.	T. Søndergaard, J. Arentoft, and M. Kristensen, “Theoretical analysis of finite-height semiconductor-on-insulator based planar photonic crystal waveguides,” J. Lightwave Technol. 20, 1619–1626 (2002). [CrossRef]
29.	M. Loncar et al., “Experimental and theoretical confirmation of Bloch-mode light propagation in planar photonic crystal waveguides,” Appl. Phys. Lett. 80, 1689–1691 (2000). [CrossRef]
30.	M. Thorhauge, L. H. Frandsen, and P. I. Borel, “Efficient Photonic Crystal Directional Couplers,” Opt. Lett. 28, 1525–1527 (2003). [CrossRef] [PubMed]
31.	S. J. McMab and Y. A. Vlasov, “SOI 2D photonic crystals for microphotonic integrated circuits,” Holey fibers and photonic crystals, (Digest of IEEE-LEOS Summer Topical Meetings, Vancouver, 2003) pp. 79–80.

OCIS Codes
(000.3860) General : Mathematical methods in physics
(000.4430) General : Numerical approximation and analysis
(130.2790) Integrated optics : Guided waves
(130.3130) Integrated optics : Integrated optics materials
(230.5440) Optical devices : Polarization-selective devices
(230.7390) Optical devices : Waveguides, planar

ToC Category:
Research Papers

History
Original Manuscript: October 30, 2003
Revised Manuscript: January 8, 2004
Published: January 26, 2004

Citation
A. Lavrinenko, P. Borel, L. Frandsen, M. Thorhauge, A. Harpøth, M. Kristensen, T. Niemi, and H. Chong, "Comprehensive FDTD modelling of photonic crystal waveguide components," Opt. Express 12, 234-248 (2004)
http://www.opticsinfobase.org/oe/abstract.cfm?URI=oe-12-2-234

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References

S. John, �??Strong localization of photons in certain disordered dielectric superlattices,�?? Phys. Rev. Lett. 58, 2486-2489 (1987). [CrossRef] [PubMed]
E. Yablonovitch, �??Inhibited spontaneous emission in solid-state physics and electronics,�?? Phys. Rev. Lett. 58, 2059-2062 (1987). [CrossRef] [PubMed]
V. P. Bykov, Radiation of atom in a resonant environment, (World Scientific, Singapore, 1993).
A. Taflove and S. C. Hagness, Computational electrodynamics: The finite-difference time-domain method, (Artech House, Boston, 2000).
S. Fan, �??Sharp asymmetric line shapes in side-coupled waveguide-cavity systems,�?? Appl. Phys. Lett. 80, 908-910 (2002). [CrossRef]
Y. Sugimoto et al., �??Fabrication and characterization of different types of two-dimensional AlGaAs photonic crystal slabs,�?? J. Appl. Phys. 91, 922-929 (2002). [CrossRef]
K. Yamada et al., �??Improved line-defect structures for photonic-crystal waveguides with high group velocity,�?? Opt. Commun. 198, 395-402 (2001). [CrossRef]
M. Loncar et al., �??Methods for controlling positions of guided modes of photonic-crystal waveguides,�?? J. Opt. Soc. Am. B 9, 1362-1368 (2001). [CrossRef]
M. Agio and C. M. Soukoulis, �??Ministop bands in single-defect photonic crystal waveguides,�?? Phys. Rev. E 64, 055603-055606 (2001). [CrossRef]
T. Ochiai and K. Sakoda, �??Dispersion relation and optical transmittance of a hexagonal photonic crystal slab,�?? Phys. Rev. B 63, 125107-125113 (2001). [CrossRef]
E. Chow et al., �??Quantitative analysis of bending efficiency in photonic-crystal waveguide bends at λ=1.55 µm wavelengths,�?? Opt. Lett. 26, 286-288 (2001). [CrossRef]
A. Chutinan and S. Noda, �??Waveguide and waveguide bends in two-dimensional photonic crystal slabs,�?? Phys. Rev. B 62, 4488-4492 (2000). [CrossRef]
A. Adibi et al., �??Properties of the slab modes in photonic crystal optical waveguides,�?? J. Lightwave Technol. 18, 1554-1564 (2000). [CrossRef]
M. Qiu and S. He, �??Numerical method for computing defect modes in two-dimensional photonic crystals with dielectric or metallic inclusions,�?? Phys. Rev. B 61, 12871-12876 (2000). [CrossRef]
Y. Sugimoto, N. Ikeda, N. Carlsson, K. Asakawa, N. Kawai, and K. Inoue, �??AlGaAs-based two-dimensional photonic crystal slab with defect waveguides for planar lightwave circuit applications,�?? IEEE J. Quantum Electron. 38, 760-769 (2002). [CrossRef]
H. Benisty et al., �??Models and measurements for the transmission of submicron-width waveguide bends defined in two-dimensional photonic crystals,�?? IEEE J. Quantum Electron. 38, 770-785 (2002). [CrossRef]
R. Ferrini, D. Leuenberger, M. Mulot, M. Qiu, J. Moosburger, M. Kamp, A. Forchel, S. Anand, and R. Houdré, �??Optical study of two-dimensional InP-based photonic crystals by internal light source technique,�?? IEEE J. Quantum Electron. 38, 786-799 (2002). [CrossRef]
A. J. Ward and J. B. Pendry, �??A program for calculating photonic band structures, Green�??s functions and transmission/ reflection coefficients using a non-orthogonal FDTD method,�?? Comput. Phys. Commun. 128, 590-621 (2000). [CrossRef]
A. J. Ward and J. B. Pendry, �??Refraction and geometry in Maxwell�??s equation,�?? J. Mod. Opt. 43, 773-793 (1996). [CrossRef]
S. D. Gedney, �??An anisotropic perfectly matched layer �?? absorbing medium for the truncation of FDTD lattices,�?? IEEE Trans. Ant. Prop. 44, 1630-1639 (1996). [CrossRef]
F. L. Teixeira and W. C. Chew, �??On causality and dynamic stability of perfectly matched layers for FDTD simulations,�?? IEEE Trans. Microw. Theory Technol. 47, 775-785 (1999). [CrossRef]
W. C. Chew and W. H. Weedon, �??A 3-D perfectly matched medium from modified Maxwell�??s equations with stretched coordinates,�?? Microw. Opt. Technol. Lett. 7, 599-604 (1994). [CrossRef]
P. G. Petropoulos, L. Zhao and A. C. Cangellaris, �??A reflectionless sponge layer absorbing boundary condition for the solution of Maxwell�??s equations with high-order staggered finite difference schemes,�?? J. Comput. Phys. 139, 184-208 (1998). [CrossRef]
S. G. Johnson and J. D. Joannopoulos, �??Block-iterative frequency-domain methods for Maxwell�??s equations in a planewave basis,�?? Opt. Express 8, 173-190 (2001), <a href="http://www.opticsexpress.org/abstract.cfm?URI=OPEX-8-3-173">http://www.opticsexpress.org/abstract.cfm?URI=OPEX-8-3-173</a> [CrossRef] [PubMed]
P. I. Borel et al., �??Efficient propagation of TM polarized light in photonic crystal components exhibiting band gaps for TE polarized light,�?? Opt. Express 11, 1757-1762 (2003), <a href=" http://www.opticsexpress.org/abstract.cfm?URI=OPEX-11-15-1757">http://www.opticsexpress.org/abstract.cfm?URI=OPEX-11-15-1757</a> [CrossRef] [PubMed]
H. Benisty et al., �??Radiation losses of waveguide-based two-dimensional photonic crystals: Positive role of the substrate,�?? Appl. Phys. Lett. 76, 532-534 (2000). [CrossRef]
J. D. Joannopoulos, R. D. Meade and J. N. Winn, Photonic crystals: Molding the flow of light, (Princeton University Press, 1995).
T. Søndergaard, J. Arentoft and M. Kristensen, �??Theoretical analysis of finite-height semiconductor-on-insulator based planar photonic crystal waveguides,�?? J. Lightwave Technol. 20, 1619-1626 (2002). [CrossRef]
M. Loncar et al., �??Experimental and theoretical confirmation of Bloch-mode light propagation in planar photonic crystal waveguides,�?? Appl. Phys. Lett. 80, 1689-1691 (2000). [CrossRef]
M. Thorhauge, L. H. Frandsen and P. I. Borel, �??Efficient Photonic Crystal Directional Couplers,�?? Opt. Lett. 28, 1525-1527 (2003). [CrossRef] [PubMed]
S. J. McMab and Y. A. Vlasov, �??SOI 2D photonic crystals for microphotonic integrated circuits,�?? Holey fibers and photonic crystals, (Digest of IEEE-LEOS Summer Topical Meetings, Vancouver, 2003) pp. 79-80.

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