We present a general approach for coupling a specific mode in a planar photonic crystal (PC) waveguide to a desired free-space mode. We apply this approach to a W1 PC waveguide by introducing small index perturbations to selectively couple a particular transverse mode to an approximately Gaussian, slowly diverging free space mode. This “perturbative photonic crystal waveguide coupler” (PPCWC) enables efficient interconversion between selectable propagating photonic crystal and free space modes with minimal design perturbations.
© 2011 Optical Society of America
Photonic crystals (PCs) exhibit a photonic bandgap that enables localization and manipulation of light at the wavelength-scale. . In two-dimensional (2D) photonic crystals, an important element is the photonic crystal waveguide, which enables compact optical delays [2, 3], slow light and enhanced nonlinear processes [4,5], and efficient connections between various on-chip devices [6–8].
Various techniques exist for coupling to photonic crystal waveguides, including chip-to-fiber butt-coupling , directional coupling from a tapered fiber [10, 11], and vertical grating couplers including slanted  or focusing lens gratings [13, 14]. Although these gratings can reach high efficiency, they constrain the PC device design as they disrupt the PC lattice and typically affect all waveguides modes. Here, we introduce a general approach for introducing highly non-invasive grating couplers that rely on small perturbations to existing device designs. For instance, in a W1 photonic crystal waveguide in a holey PC membrane, the grating consists only of small dielectric index perturbations to a set of holes near the waveguide region. We call this coupling device a Perturbative Photonic Crystal Waveguide Coupler (PPCWC). Although this approach is general, we focus here on the situation where we introduce extra holes adjacent to the existing air holes. This restricted set of perturbations eliminates fabrication challenges that may be associated with non-circular or very small, isolated perturbations.
Similar directional coupling from photonic crystal cavities by introducing small perturbation has been explored in previous studies [15–17]. The index perturbation is derived here using coupled mode theory, under the constraint that it can be easily integrated into the photonic crystal fabrication. This approach enables a straightforward design of perturbations that causes selective coupling between a desired PC waveguide mode and a desired free-space mode (chosen here to be a Gaussian). Figure 1(a) shows the coupling scheme. When light propagates along the waveguide (the red arrows) and passes through the coupler, the periodic index perturbations act as a grating and light scatters out of the slab. We use three-dimensional finite difference time domain (FDTD) simulations to calculate the waveguide modes for a given index perturbation and to find the efficiency of the resulting grating coupler. We find that even very small perturbations allow a high coupling efficiency between the free-space radiative mode and a given waveguide mode, while causing only very small changes to the propagation of other waveguide modes. As demonstrated in the end of Section 2, the directional scattering from this coupler is controllable by detuning the feed frequency or modulating the perturbation size. In Section 3, we discuss the mode selectivity of our device by investigating the problem in k-space, and in Section 4 we analyze the transmittance and the modification of the shape and the directionality of the scattered beam.
2. Coupled mode theory
We consider a guided wave in a W1 photonic crystal line defect waveguide and the light scattered at the grating coupler. We derive the coupled mode equations from wave equationEq. (1) with ɛ = ɛw is in form of
B⃗w are Bloch states having periodicities as the multiples of the periodicity of ɛw, where k⃗ represents the crystal momentum and x̂ is the propagating direction of the waveguide. We desire a scattered beam propagating in free space denoted by A⃗(r⃗). A⃗ is also a solution of Eq. (1) with the relative dielectric constant ɛ = ɛG. We assume the field to be a superposition of the waveguide and free space modes:
Here, a(t) is the slowly varying component of the Gaussian beam, and b(k⃗,t) and c(k⃗,t) are the slowly varying components of the forward and backward propagating Bloch modes for the waveguide, respectively. Substituting Eq. (3) into Eq. (1), we can obtain the full coupled mode equations describing the interaction of the coefficients a(t), b(k⃗,t), and c(k⃗,t) through Δɛ. In particular, the coupling rate between a(t) and b(k⃗,t) can be evaluated [7,19] to be
From Eq. (4), the coupling constant is determined by A⃗* · B⃗k⃗ and the perturbation term Δɛw. Since the phase of A is nearly constant in the plane of the PC, whereas B⃗k⃗ varies rapidly along the direction of propagation, the spatial integral of the dot product A⃗* · B⃗k⃗ will vanish. For a non-vanishing coupling constant, the index perturbation Δɛw should have the same periodicity as B⃗k⃗, assuming an interaction region that is large compared to the period a.
Now we consider a realistic waveguide made by introducing a line defect in a hexagonal photonic crystal lattice with periodicity a, refractive index of the slab material n = 3.6, slab thickness h = 0.7a, and hole radius r = 0.3a. The full coupling system is as shown in Fig. 1(a). We used a 3D FDTD simulation to calculate the waveguide modes. Figure 1(b) shows the dispersion relation of the W1 photonic crystal waveguide. A fundamental and higher order mode inside the photonic bandgap (PBG), wedged by the areas shaded in gray, are shown in blue and green, respectively, and are confined below the light line, represented by the red line. Figures 2(a) and 2(b) show the x̂ and ŷ electric field components of the fundamental mode, which we label as B⃗k⃗, at wave-vector kx = π/a, and frequency ω = 0.2436, in units of 2πc/a, where c is the speed of light in free space. As shown previously, the index perturbation must have a period of 2π/k⃗x = 2ax̂ to scatter this k-state to the point in k-space, where the in-plane kx = 0. Note that because the x̂ and ŷ components of the electric field of the waveguide mode have different symmetries along the ŷ direction, an index perturbation with even symmetry across y = 0 will scatter only the ŷ-component, but not the x̂-component of the field. Similarly, it is possible to scatter only the x̂-component with a anti-symmetric perturbation distribution across the y = 0 line. For the following analysis, we will choose to scatter the ŷ-component. Furthermore, we suppose that we want to scatter into a vertical mode that has a Gaussian profile in the in-plane directions, as shown in Fig. 2(c). Figure 2(d) shows the dot product A⃗* · B⃗k⃗,y, which appears in the integrand in Eq. (4). To find a perturbation that scatters light into a slowly diverging Gaussian beam, we calculate the coupling rate for beams with different divergence angles and compare the coupling constants among different index perturbation designs. We discuss in this paper, the perturbations are formed by enlarging three-hole clusters with periodicity 2a in the x̂-direction. The blue and green lines in Fig. 2(e) represent the coupling constants κ1 and κ2 for Gaussian beams, focused in the plane of the photonic crystal, with waists of 2a and a, respectively, and the red line represents the ratio κ1/κ2. The horizontal axis denotes the perturbation size in units of the area of the unit cell of the triangular lattice, and the vertical axes denote the coupling constant (left) and the ratio κ1/κ2 (right). We observe that a local maximum exists for κ1/κ2 when the index perturbation size is 0.3244, in units of the fractional area of unit cell, that is, the light scattered in this case diverges less than a well-defined Gaussian beam. The perturbed structure for this case is shown in Fig. 2(f) and the corresponding coupling strength κ1 and the ratio κ1/κ2 are 0.2228 and 1.815, respectively. As expected, the coupling rate into the Gaussian beam of smaller waist is lower than for the wider, less rapidly diverging beam. The brown shaded area in the right panel of Fig. 2(f) shows the index perturbation.
We check our theoretical predictions using another 3D FDTD simulation of the coupling efficiency of a grating consisting of the index perturbation as shown in Fig. 2(f). The fundamental waveguide mode at frequency ω = 0.2436 is excited by a Gaussian beam source at one end of the PC waveguide. The ŷ-component of the electric field in the plane of the PC is shown in Fig. 3(a), which contains five periods of the index perturbation shown in Fig. 2(f). The perturbation couples the incident waveguide mode upward, resulting in reduced waveguide transmission (< 0.5%) on the right side of the perturbation. In Fig. 3(b), we consider the effect of this perturbation on a higher-frequency mode at ω = 0.3078, which also has even symmetry across the y = 0 axis, but which has a periodicity of a in the direction of propagation. Equation (4) predicts that if Δɛ has a periodicity of 2a, the coupling constant κba will vanish in this case. This result is confirmed by a high in-plane transmission after the coupler (> 99%), as shown in Fig. 3(b). We will discuss this mode selective property of the coupler in greater detail in Section 3.
Figure 4 displays the energy density of the y⃗ component of the evanescent field and the upward component of the scattering field from the coupler. Figure 4(a) is a snapshot viewed in the vertical cross-section through a plane passing through the middle of waveguides, and Fig. 4(b) is the three dimensional view of the Ey energy density isosurface. We observe a strong radiated field originating from the 5-period long perturbed region.
As observed in Fig. 4, the radiation exits at 43° from the vertical. This direction depends on the interference of the fields scattered by discrete perturbations, as in a line grating. The interference is governed by relative amplitudes and phases of the fields at the positions of the perturbations. The scattered field can be approximated as a sum over all perturbations:Eq. (5) includes the decrease of the field amplitude along the coupler, α, and the phase difference of the waveguide mode between perturbations. Because the perturbations are r⃗i have a periodicity of 2ax̂, the phase difference is equivalent to 2aΔkw,x. Equation (5) therefore predicts a shifting of the diffraction angle with wavelength, as given by the waveguide’s dispersion relation. We observe this dependence in numerical simulations. In Fig. 5(a), the frequency of the incident waveguide mode is tuned from ω = 0.2960 to ω = 0.3120 as the scattering angle shifts from −4° to 20°.
The coupled mode theory discussed above assumes a weak perturbation to the waveguide mode. However, the mode intensity drops as the field propagates through the coupler. This decrease in mode intensity should be taken into account to improve the efficiency of the coupler. Figure 5(b) shows the structure of a 5-period long coupler in which we now include an increasing perturbation size to compensate for the decreasing field intensity. Using Eq. (5,6) to estimate the field intensity profile along the waveguide, we simulate a 5-period long coupler with perturbation sizes multiplied by factors of 0.8589, 0.8973, 0.9059, 0.9731, and 1. Figure 5(c) shows the resulting intensity distribution of the scattered field viewed in a vertical plane through the center of the waveguides. We now observe a more uniform scattering along the length of the perturbation coupler, which results in higher mode overlap with the vertical Gaussian beam.
3. Mode selectivity
It is clear from the coupled mode picture that the out-coupling rate from the waveguide depends on the in-plane periodicity and the symmetry of the waveguide mode; for example, as was shown in Fig. 3, the in-plane transmission after the coupler is suppressed for the fundamental mode, but not for the higher-order mode at ω = 0.3078. We now analyze this mode selectivity more closely in k-space. Figure 6(a) compares the dispersion relations for the fundamental mode (the blue line) and a higher mode (the green line) inside the photonic band gap, having frequencies of ωA = 0.2436(2πc/a) and ωB = 0.3151 at kx = π/a. For the structure with index perturbations (the right panel), the dispersion is raised slightly because of the decrease in the effective refractive index. The periodicity of 2a scatters modes near kx = π/a by a lattice vector of Δkx = π/a to the point where kx = 0. Since these components are above the light line, they leak out of the PC plane and result in higher loss rate of the waveguide mode.
In Fig. 6(b), the blue line shows the loss rate, γr, normalized by the loss rate of the fundamental waveguide mode in the unperturbed structure, through different perturbation patterns. The green line shows γr for the higher-order waveguide mode at ω = 0.3151. As the perturbation size increases, the loss rate of the fundamental mode increases by over two orders of magnitude, while the loss rate of the higher-mode remains roughly constant. This result demonstrates a high degree of selectivity of the perturbation coupler between different kinds of waveguide modes. Figure 6(c) shows the frequency increase of the fundamental and higher order mode (the blue and green lines).
4. Transmittance and beam shape modification
The efficiency of the coupler is estimated by calculating the transmittance from the waveguide mode to a target free space Gaussian spatial mode, which includes both upward and downward components. We approximate the efficiency byFig. 7 (the red solid line). The perturbations not only scatter the incident waveguide mode into the Gaussian mode, but also induce backward reflection (the gray solid line) and other in-plane leakage (the gray dotted line). The maximal scattering rate is reached when r0 = 0 and the perturbation size in the sides is 0.4466, in units of the fractional area of unit cell. As shown in Fig. 7, the scattering rate doubles when the perturbation size increases about 40% (the region A), but slightly decreases as the radius of the central holes increases (the region B). If a perturbation is introduced only at the center of the waveguide (the region C in Fig. 7), then the incident light is mostly reflected and only weakly scattered out of plane.
When coupling to free space optics, and especially for single mode fiber coupling, the scattered field should have a large overlap with a Gaussian mode. In the case with the maximal scattering rate of 0.6989, we calculate an overlap of 89% with a Gaussian beam focused in the plane of the PC. This indicates that the coupler allows for both strong scattering and a highly Gaussian-like profile. The resulting transmittance through the coupler is Tc = 0.6989 × 89% = 62%.
It is possible to decrease the beam divergence to allow for coupling to lower-NA lenses. By increasing the extent of the PPCWC in both x̂ and ŷ (transverse in-plane direction), we expand the coupling region and decrease the output beam divergence. This modified index perturbation is shown in Fig. 8(a), again optimized for the mode at ω = 0.2436. Figures 8(b) and 8(c) show the intensity distributions of beams scattered from a small coupler (Fig. 3) and a broadened one (Fig. 8(a)), viewed in y–z plane through the centers of the couplers. Figures 8(d) and 8(e) compare the divergence of the radiated beams in both cases by fitting a Gaussian beam profile to the data. We assume 2θ = 2W0/z0, where 2θ is the divergence angle of the beam and W0 and z0 are the beam waist and depth of the focus, respectively. In the case of the broadened coupler, the divergence is decreased by 20% from that of the original smaller coupler.
Unfortunately, the out-of-plane scattering from the PPCWC is symmetrically upward and downward, so both contribute to the total scattering rate. While large Tc can be achieved by the methods described above, the overall efficiency of the PPCWC is so far limited to 50%. The upward scattering efficiency is defined as the directionality,15,17] and channel waveguides .
We have designed and implemented a method for selectively coupling a planar photonic crystal waveguide mode to a target free space mode. The method proceeds as follows: (1) one chooses a waveguide mode to out-couple, (2) one chooses an index perturbation to couple the mode that has the appropriate periodicity and symmetry given by coupled mode theory, and finally, (3) one optimizes the perturbation for the desired out-coupled beam parameters. To demonstrate this approach, we focused on the problem of coupling a W1 waveguide mode to a slowly diverging Gaussian mode. We were able to ensure that the target waveguide mode was coupled with high rate, selectivity, and overlap with the target Gaussian mode.
This perturbative photonic crystal waveguide coupler (PPCWC) not only enables efficient scattering of selected waveguide modes, but also allows modifications in the shape and the direction of scattering. The angle of the scattered field can be shifted by detuning the mode frequency with respect to the lattice constant or introducing some modulation to the perturbation size. By breaking the vertical symmetry of the PC or using reflectors under the PC slab, it is possible to minimize downward propagation, directing most vertical scattering upward. The PPCWC enables a straightforward integration of vertical in/out- couplers which can be employed in a range of application from optical interconnects to photonic crystal light sources. Furthermore, the spectrally resolved light coupler could find application in light trapping for thin-film solar photovoltaics.
C.C.T. was partially supported by the Center for Re-Defining Photovoltaic Efficiency Through Molecule Scale Control, an Energy Frontier Research Center funded by the U.S. Department of Energy, Office of Science, Office of Basic Energy Sciences under Award Number DE-SC0001085. J.M. was supported by the DARPA Information in a Photon program, through grant W911NF-10-1-0416 from the Army Research Office.
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