An optical spectral singularity is a zero-width resonance that corresponds to lasing at threshold gain. Its time-reversal causes coherent perfect absorption of light and forms the theoretical basis of antilasing. In this article, we explore optical spectral singularities of a two-layer spherical medium. In particular, we examine the cases that a gain medium is coated by a thin layer of high-refractive index glass and a spherical glass covered by a layer of gain material. In the former case, the coating reduces the minimum radius required for exciting spectral singularities and gives rise to the formation of clusters of spectral singularities separated by wide spectral gaps. In the latter case, the coating leads to a doubling of the number of spectral singularities.
The discovery (Mostafazadeh 2009a) that the mathematical concept of a spectral singularity (Naimark 1954, for a recent review, see Guseinov 2009) has physical realizations as zero-width resonances of complex scattering potentials has motivated a detailed study of this phenomenon (Ahmed 2009; Longhi 2009; Mostafazadeh 2009b; Andrianov et al. 2010; Longhi 2010a,b,c, 2011a; Mostafazadeh 2011a,b,c; Mostafazadeh & Sarisaman 2011; Samsonov 2011). In particular, it is shown that optical spectral singularities (OSS) correspond to the lasing at the threshold gain (Mostafazadeh 2011a) and that a time-reversed OSS (Longhi 2010b,c, 2011a) yields a coherent perfect absorption (CPA) of light, i.e. an antilasing (Chong et al. 2010; ; Chong et al. 2011; Ge et al. 2011; Longhi ; Wan et al. 2011).
Typical lasers are photonic devices consisting of an active medium placed inside an optical cavity. A particularly interesting type of lasers are those based on spherical granules where the surface of the sphere acts as the cavity (Alexopoulos & Uzunoglu 1978; Kerker 1978; Benner et al. 1980; van de Hulst 1981; Bohren & Huffman 1983; Sandoghdar et al. 1996; Sasaki et al. 1997; Gorodetsky & Ilchenko 1999; Takahashi et al. 1999; von Klitzing et al. 2001; Vahala 2003). These are characterized by their extremely high-quality factors and small volumes of excitation. Owing to these properties, a spherical laser can also be realized in which the active medium is located outside an spherical core (Matsko et al. 2005; Matsko & Ilchenko 2006).
In Mostafazadeh & Sarisaman (2011), we studied the OSS of a uniform spherical gain medium and showed for the radial (transverse) modes of a concrete spherical dye laser that the emergence of an OSS puts a lower bound on the radius of the gain medium. This is the minimum radius required for lasing in these modes. In the present article, we examine OSS and CPA for an active medium consisting of a spherical inner core and a spherical outer shell with different refractive indices, as shown in figure 1. In particular, we wish to explore the prospects of reducing the value of by means of coating the spherical gain medium by a material with higher refractive index.1
2. Radial transverse spherical electromagnetic waves
Consider an optically active material with an inner spherical core of radius a1 and an outer spherical shell of thickness a2−a1 placed in a vacuum. Let and denote the complex refractive indices of the inner core and the outer shell, respectively, and suppose that they are independent of space and time. The electromagnetic (EM) waves interacting with this system satisfy the Maxwell equations: 2.1 and 2.2 where , , ε0 and μ0 are, respectively, the permeability and permittivity of the vacuum, r:=|r| is the radial spherical coordinate, 2.3 and each over-dot represents a time-derivative. According to (2.2), the electric field E=E(r,t) is a solution of the wave equation: 2.4 where and c=(ε0μ0)−1/2 is the speed of light in vacuum.
For a time-harmonic EM field with angular frequency ω that propagates in a charge-free medium, we have E(r,t)=e−iωtE(r), and (2.4) reduces to the time-independent Schrödinger equation 2.5 where k:=ω/c is the wavenumber and v is the complex barrier potential: .2
Following the analysis of Mostafazadeh & Sarisaman (2011), we investigate transverse radially propagating spherical solutions of (2.5) that have the form 2.6 Here is the unit vector associated with the azimuthal angular coordinate ϕ of the spherical coordinate system. Inserting (2.6) in (2.5) yields 2.7 For r<a1, a1<r<a2 and r>a2, where v takes constant values, we can transform (2.7) to the spherical Bessel equation of order , (Jackson 1975). Therefore, 2.8 where the Ai and Bi are constant numerical coefficients, jν,nν and are, respectively, the spherical Bessel, Neumann and Hankel functions, and for i=1,2. Notice that the condition that the electric field be regular at the origin implies that B1=0. Consequently, E(0)=0.
Having obtained the explicit form of the electric field, we can compute the magnetic field using (2.2). This gives 2.9 where is the unit vector associated with the spherical polar coordinate θ, 2.10 and for each differentiable function f we define according to . Notice that for every pair of differentiable functions and positive real numbers , 2.11 Because this quantity will frequently appear in our calculations, we denote it by for brevity. In other words, 2.12 Recall that the Wronskian of f and g is given by . Therefore, 2.13
In order to relate the coefficients Aj and Bj appearing in (2.8), we need to impose the appropriate matching conditions at the boundaries r=a1 and r=a2, (Jackson 1975). For the system we consider, these correspond to the condition that the parallel component of both the electric and magnetic fields must be continuous at the boundaries. In view of (2.6) and (2.9), this means that E=E(r) and B=B(r) must be continuous functions. We can satisfy this condition provided that we select the coefficients Ai and Bi such that E and B are continuous at r=a1 and r=a2. This gives 2.14 where for all p,q=1,2, 2.15 According to these equations and (2.13), 2.16 and 2.17 The fact that these quantities do not vanish was to be expected, because (jν,nν) and (h(1),h(2)) are pairs of linearly independent solutions of a second-order homogeneous linear differential equation. Equations (2.16) and (2.17) imply that Kpq and L are invertible matrices. We can use their inverse together with equation (2.14) and the fact that A1≠0, to express A3 and B3 in terms of A1 according to A3=M11A1 and B3=M21A1, where Mij are the entries of the transfer matrix 2.18
3. Optical spectral singularities and coherent perfect absorption for radial transverse spherical waves
As discussed in Mostafazadeh & Sarisaman (2011), we can easily exploit the asymptotic properties of the spherical Hankel functions to infer that the reflection amplitude of our system is given by 3.1 Therefore, in order to characterize OSS and CPA that correspond to the real poles and zeros of R, we only need to calculate M11 and M21. Using (2.11), (2.16), (2.17), (2.12), (2.15), (2.18) and doing the necessary algebra, we obtain 3.2 where for both ℓ=1,2, 3.3 and 3.4 In view of (3.2)–(3.4) and the fact that , we can express (3.1) in the form
Equations (3.2) provide a simple demonstration of the fact that CPA corresponds to an OSS of the time-reversed system. To see this, we recall that we can obtain the time-reversed system by complex-conjugating the refractive indices . This implies 3.5 and 3.6 where we have used (3.3), (3.4), (3.2), (3.1) and the fact that . According to the last relation in (3.6), a CPA, that corresponds to R=0, appears if and only if the reflection coefficient of the time-reversed system diverges, i.e. the latter develops an OSS and begins lasing at the threshold gain. Therefore, in the following, we only consider the problem of locating OSS. We can easily obtain the values of the physical parameters leading to a CPA of the spherical waves we consider by complex-conjugating the refractive indices and or changing the sign of the gain/attenuation coefficients of both the layers.
A straightforward consequence of this observation is the fact that because the law of energy conservation prohibits the emergence of an OSS for the case that both the interior core and the outer shell of our system consist of lossy material, a CPA cannot be realized unless either the core or the outer shell includes a lossy medium. Furthermore, it is possible to generate both a CPA and an OSS, if our system involves both lossy and gain media.
In order to determine the location of OSS in the space of the physical parameters of the system, we study the real zeros of M21 or alternatively N1 in the complex k-plane. In view of (3.3) and (3.4), this is equivalent to finding the real values of k fulfilling 3.7 Noting that , this is a complex transcendental equation involving two complex variables, namely and , and two (positive) real variables: x1:=ka1 and x2:=ka2.
For a1=a2 and that corresponds to a homogeneous spherical medium that we consider in Mostafazadeh & Sarisaman (2011), the first factor on the left-hand side of (3.7) vanished identically and the first factor on its right-hand side becomes W[nν(x),jν(x)] with . Because the latter is non-zero, (3.7) reduces to 3.8 We can use the identity 3.9 to express the derivative of the spherical Bessel, Neumann and Hankel functions. Doing this in (3.8) gives rise to the equation for the spectral singularities of a spherical gain medium that we derive in Mostafazadeh & Sarisaman (2011), namely 3.10
Employing the identity (3.9) in (3.7) gives a more lengthy equation for OSS that we use in our numerical and graphical investigations. Before reporting the results of this investigation, however, we will carry out a perturbative analysis of (3.7). Similarly to the single-layer spherical medium, we studied in Mostafazadeh & Sarisaman (2011), this turns out to reveal some basic properties of the solutions.
4. Perturbative analysis of optical spectral singularities
Consider the Mie regime where a2≥a1≫2π/k=:λ and . Then x2≥x1≫1, , and we can perform a large-x1 (and -x2) expansion of the terms appearing in (3.7). This requires using the following asymptotic expansions of the spherical Bessel, Neumann and Hankel functions. 4.1 4.2 4.3 where and Γ stands for the Gamma function.
Substituting (4.1)–(4.3) in (3.7), neglecting the quadratic and higher order terms in and in the resulting equation, noting that and , and introducing 4.4 and 4.5 we find 4.6 where we use ‘≈’ to indicate that this equation is obtained by employing first-order perturbation theory. Solving (4.6) for x2 yields 4.7 where we have used ‘’ to denote the principal part of natural logarithm of its argument, suppressed the argument of for brevity, and employed the identity 4.8 The parameter m appearing in (4.7) is an integer that we identify with a mode number labelling OSS.
Because the left-hand side of (4.7) is real, we can express this complex equation as a pair of real equations 4.10 and 4.11 We also note that 4.12
Next, we consider the special case of a coated spherical active medium with a2−a1≪a1. In this case, the gain/absorption properties of the coating can be neglected and may be assumed to take a real value that we label by n2. This implies the equivalence of (4.11) and the condition that the absolute value of (4.12) must be unity. Imposing this condition and noting that in this case is also real, we find 4.13 This is a real equation involving a complex variable, , and two real variables, n2 and x1. In particular, it does not involve the mode number m.
In order to use (4.13) for locating OSS, we express and in terms of their real and imaginary parts. Let η1 and κ1 denote the real and imaginary parts of , so that 4.14 and introduce 4.15 Then substituting (4.14) in (4.4) gives 4.16
Next, we use (4.14), (4.16) and various trigonometric and hyperbolic identities to obtain the following explicit form of (4.13). 4.17 A similar analysis reveals the fact that the following quantity is an integer. 4.18 where 4.19 and 4.20 and ‘arg(z)’ denotes the principal argument of z that takes values in (−π,π]. The latter implies that is one of the two integers satisfying the condition: 4.21 A more important implication of (4.18) is that it leads to the following explicit form of (4.10). 4.22 where 4.23 Note that the ‘’ appearing in (4.20) stands for the principal value of ‘’ that takes values in [−π/2,π/2]. This in particular implies that . Therefore, 4.24 Another useful relation that follows from (4.19), (4.20) and (4.23) is 4.25
Equation (4.22) is quite remarkable, for it indicates that if we choose η1,κ1,n2 and x1=2πa1/λ, so that x1≫1 and (4.17) holds, then an OSS arises for a discrete set of values of the thickness of the coating. Because is an integer, according to (4.22) and (4.24), 4.26 This means that the mode number m and the thickness a2−a1 are bounded from below by (γ−1)/2 and λ/(8n2), respectively. Notice that these bounds only depend on a1, λ and n2.
Next, we examine the physical implications of (4.17) for a typical optically active material that satisfies 4.27 In this case, we can ignore the terms of order two and higher in κ1 and β in our calculations. Implementing this approximation in (4.17), using (4.15), and recalling that the imaginary part of , i.e. κ1 is related to the gain coefficient g via κ1=−gλ/(4π), we find 4.28 This relation shows that the radius a1 of the inner core is inversely proportional to the gain coefficient. Furthermore, it puts curious upper and lower bounds on the possible values of a1 that are only sensitive to the gain coefficient and the real part of the refractive indices of the inner core and the outer shell: 4.29 where and are, respectively, the largest and smallest of η1 and n2.
In view of (4.29), the larger n2 is, the smaller the lower bound of a1 gets. This confirms our expectation that coating a spherical gain medium by a material with higher refractive index reduces the lower bound on the radius of the gain medium. For example, if we take n2=2.5 and choose the inner core to be made of a dye gain material with η1≈1.48 and g≈5 cm−1, we find 4.30
Finally, we explore the consequences of (4.27). Implementing the above approximation scheme of neglecting second and higher order terms in β and κ1 in (4.22) yields 4.31 Taking a1=1 mm to comply with (4.30), choosing λ=549 nm, η1≈1.48 and n2=2.5 as above, and using (4.22), (4.19), (4.21), (4.26) and (4.31), we find 4.32 The smallest allowed value of the thickness is therefore a2−a1≈a0=27 nm.
In practice, the thickness of the coating has a fixed value, and (4.31) and (4.32) determine an approximate value of the mode number m: 4.33 If we further approximate by γ and use the expression (4.25) for the latter, then (4.33) gives 4.34 For example, for a2−a1=5 μm, this relation gives m≈9152, which coincides with the numerical result obtained directly from (4.10).
We can also use (4.34) to express the wavelength of the OSS in terms of the mode number. This gives 4.35 The analogous expression for the case that we remove the coating is given by eqn (33) of Mostafazadeh & Sarisaman (2011) and reads 4.36 Comparing (4.35) with (4.36) and noting that n2a2>η1a1, we can see that the presence of the coating increases the wavelength of the OSS associated for each mode number. Alternatively, it increases the value of the mode number for an OSS of a given wavelength.
We conclude this section by pointing out that we can perform a perturbative calculation of OSS in a way that avoids the explicit appearance of the mode number m. According to (4.22) and (4.23), . In light of (4.20), we can easily compute and express the latter equation in the form 4.37 In summary, we have obtained the real equations (4.17) and (4.37) by imposing the complex equation (4.6). We derived the latter by performing first-order perturbation theory on (3.7) that determined OSS. It is important to note that every solution of (4.6) is a solution of (4.17) and (4.37), but the converse may not be true. We have checked for some concrete examples and found that indeed this is the case. Therefore, we solve (4.17) and (4.37) by fixing all but two of the real parameters entering in these equations and then eliminate the solutions that violate (4.6).
5. Optical spectral singularities of a concrete two-layer spherical medium
In general, the refractive index of an optically active medium depends on the properties of the medium and the wavelength of the propagating EM wave. For example, for a gain medium that is obtained by doping a host medium of refraction index n0 and modelled by a two-level atomic system with lower and upper level population densities Nl and Nu, resonance frequency ω0 and damping coefficient γ, it satisfies the dispersion relation (Mostafazadeh 2011a): 5.1 where , , , e is the electron's charge, and me is its mass. We can express in terms of the imaginary part κ0 of at the resonance wavelength λ0:=2πc/ω0 according to Mostafazadeh (2011a) 5.2 where the approximation symbol means that we neglect quadratic and higher order terms in κ0.
Inserting (5.2) in (5.1) and using , we obtain 5.3 where 5.4 We also note that the gain coefficient of such a medium is given by g=−4πκ/λ. In particular, we can use this relation to express κ0 in terms of the gain coefficient g0 at the resonance wavelength λ0 according to 5.5 In the following, we employ (5.3)–(5.5) to parameterize the refractive indices and that enter in the description of our two-layer spherical model.
In order to explore the effect of the outer shell on the behaviour of spectral singularities, we consider a spherical dye laser medium confined in a thin spherical shell of higher refractive index glass. We suppose that the refractive index of the glass takes a constant real value and parameterize the location of the spectral singularities using the resonance gain coefficient, g0, of the dye and the wavelength λ.
Consider confining a Rose Bengal-dimethyl sulphoxide (DMSO) solution with characteristics (Silfvast 1996; Nooraldeen et al. 2009) 5.6 in a spherical glass shell of outer radius a2=1 mm, thickness a2−a1=5 μm and refractive index n2=2.5.3 Figure 2 and table 1 show the results of our numerical calculation of the location of spectral singularities that use (3.7).
Table 1 also gives the results of our perturbative calculations and demonstrates their good agreement with the numerical results.
Let denote the smallest value of the gain coefficient g0 that is capable of producing an OSS, and λ(1) be the wavelength of this OSS. We recall from Mostafazadeh & Sarisaman (2011) that in the absence of coating λ(1) is essentially identical with the resonance wavelength λ0. According to figure 2 and table 1, the presence of the glass coating causes λ(1) to be slightly red-shifted.
Figure 3 shows a logarithmic plot of the reflection coefficient as a function of the wavelength for the sample considered in figure 2 and table 1 with . In this case, there is an OSS at λ=λ(3)=549.56092702 nm that corresponds to the central peak in figure 3. Unlike the other peaks shown in this figure, the height of the central peak increases indefinitely as we use more and more accurate numerical values for the parameters of the system. This is a clear indication that it corresponds to a spectral singularity.
Next, we explore the effect of changing the thickness of coating a2−a1 on the λ(1) while keeping the inner radius fixed. Figure 4 shows the graph of λ(1) as a function of thickness. As seen from this figure, as we increase the thickness, λ(1) undergos an infinite set of jumps that oscillate about the resonance wavelength λ0 with a decreasing amplitude. Our numerical results show that unlike the wavelength λ(1), the gain coefficient does not experience a noticeable change owing to an increase in the thickness.
Figure 5 shows the location of OSS for a spherical dye gain medium without a coating. Comparing this figure with figure 2, we see that except for the shift in the value of λ(1), the distribution of the OSS in the λ−g0 plane does not seem to get affected by the presence of the coating glass. Exploring a wider range of values of λ and g0 reveals a different picture. Figures 6 and 7 show the location of OSS in a wider spectral range for a coated spherical Rose Bengal-DMSO sample with specifics (5.6), inner radius 1.5 mm, and two different values of the coating thickness, namely 5 and 10 μm. As these figures show, OSS are located on curves with multiple local minima. The number of these minima that fulfill the experimental upper bound of g0≤5 cm−1 is an increasing function of the thickness of the coating. For a2−a1=5 μm (figure 6), this number is three, i.e. there are three distinct groups of OSS satisfying the bound: g0≤5 cm−1. These appear in the spectral ranges 536.941436–539.544783, 546.335226–552.571190 and 560.400334–561.815048 nm and, respectively, contain 41, 93 and 21 members. Their central member that corresponds to the smallest gain coefficient appear at (λ,g0)=(538.239847,4.601744),(549.435560,3.218290) and (561.106835,4.895167) in (nm,cm−1) units. For a2−a1=10 μm (figure 7), there are four groups of OSS satisfying the bound on g0. They include 34, 47, 46 and 30 members with wavelengths ranging over 539.621948–541.782279 nm, 544.992898–548.067753 nm, 550.878022–553.951299 nm and 557.516880–559.542755 nm, respectively. The central members of these four groups that correspond to the local minima of g0 have (λ,g0) values: (540.666848,4.010267), (546.525852,3.287748), (552.444850,3.348007) and (558.493430,4.217539) in (nm,cm−1) units. In particular, the presence of the glass coating not only allows for generating OSS in a smaller gain medium, but it produces spectral gaps in the spectral range within which these OSS are located. These remarkable observations should, in principle, be verifiable experimentally.
Next, we study the effect of changing the radius of the inner core on the location of OSS for a fixed value of the coating thickness. Figure 8 shows the graph of the minimum gain coefficient g0 necessary for generating an OSS as a function of a1 for the coated spherical Rose Bengal-DMSO dye gain medium with specifications (5.6) and thickness 5 μm. For , no OSS can be created. Recalling that for an uncoated sample , this corresponds to a threefold decrease in the size of the gain medium. As we increase a1 starting from the critical value 0.96 mm, the minimum gain coefficient necessary for generating an OSS, namely decreases. Both of these observations are in agreement with our perturbative results. Moreover, it turns out that for fixed values of the coating thickness, the wavelength λ(1) is not sensitive to the variations of the inner radius. Figure 9 demonstrates this behaviour. As our perturbative treatment shows the larger the refractive index of coating is the smaller the minimum radius gets. For example, if we use a glass coating with the same thickness (5 μm) but a slightly lower index of refraction, say n2=1.93 as in Shibata et al. (2006), the value of increases by a factor of 2 (to about 1.8 mm).
We have also investigated the formation of OSS in a two-layer spherical model in which the inner core is made of a higher refractive index glass and the outer shell is filled with a dye gain material. Using the same glass and gain material and taking the core radius to be 2 mm, we found that the minimum shell thickness required for producing an OSS was about 3.28 mm. This coincides with the minimum radius supporting an OSS for a sphere filled with the same gain material. Figure 10 shows the location of OSS for the thickness of 3.3 mm as given by (3.7). The main difference between this figure and figure 5 is that the number of OSS has doubled. To our knowledge, this is the only effect of the presence of the glass core. We also find that using a glass core with a lower index of refraction does not have a sizable effect on the location and number of OSS.
6. Concluding remarks
A gain medium can emit EM waves provided that we adjust its parameters so that an OSS is created. The time-reversal of this phenomenon corresponds to the (coherent perfect) absorption of EM waves. This is the theoretical basis of antilasing. The simplest example of a gain medium that is localized in space and is capable of realizing an OSS is a spherical gain medium. It supports spectral singularities in a radial transverse mode provided that its radius exceeds a critical value .
For the typical dye laser material that we consider in Mostafazadeh & Sarisaman (2011), mm. In practice, maintaining a uniform gain coefficient within a spherical sample of this size can be difficult. The main motivation for the current study is the idea that coating a spherical gain medium by a high-refractive index material can reduce . We have shown by explicit perturbative and numerical calculations that this is actually the case. In particular, coating a spherical active dye medium with a glass of thickness 5 μm and index of refraction 2.5 reduces by about a factor of 3. Furthermore, we have found that the presence of coating leads to a much richer structure as far as the location of spectral singularities are concerned. In particular, the coating causes a small shift in the wavelength of the spectral singularity that requires the least amount of gain. More importantly, it produces a clustering of spectral singularities into groups separated by sizable spectral gaps. This behaviour may find an application in producing tunable lasers with rather wide spectral gaps. Another interesting possibility is to generate laser pulses in different spectral ranges by periodically altering the gain coefficients of the active core. For example, as shown in figures 6 and 8, increasing the gain coefficient so that it passes one or more of the local minima of the OSS curves leads to lasing in two or more spectral ranges that are separated by gaps of several nanometres in width.4
If we use a glass spherical core and an active dye outer shell, the thickness of the shell required to induce an OSS is about the for an uncoated spherical gain medium consisting of the same dye. The presence of the glass core does not seem to have a significant effect except for the doubling of the number of spectral singularities. We plan to explore the reasons for this phenomenon in a more general context.
The results we have reported apply for a transverse electromagnetic (TEM) wave propagating in the radial direction. As we show in the appendix, we can extend our investigation to study OSS for EM waves in the transverse electric (TE) and transverse magnetic (TM) modes. It turns out that the results are similar to those for the TEM mode. For example, the size of the remains essentially the same.
The emergence of an optical spectral singularity is a common feature of any lasing system. This includes typical coated or uncoated spherical lasers that can be realized using much smaller, micrometre size dye samples (Datsuyk et al. 2005; Shibata et al. 2006; Beltaos & Meldrum 2007; Dantham & Bisht 2009; Xiao et al. 2010). The reason is that these lasers involve exciting whispering gallery modes (Matsko et al. 2005; Matsko & Ilchenko 2006). We intend to conduct a through study of optical spectral singularities for whispering gallery modes.
We wish to express our gratitude to Ali Serpengüzel for reading the draft of this article and making many useful comments and suggestions. This work has been supported by the Scientific and Technological Research Council of Turkey (TÜBİTAK) in the framework of the project no. 110T611 and the Turkish Academy of Sciences (TÜBA).
In this appendix, we extend our analysis of optical spectral singularities to the general TE(ℓ,m) and TM(ℓ,m) modes of our two-layer spherical system.
We begin our treatment by writing the solutions of the Maxwell's equations in TE and TM modes of a spherical system as follows (Jackson 1975): A 1 and A 2 where ℓ and m take integer values in ranges and [−ℓ,ℓ], respectively, aE and aM are the coefficients of TE and TM modes, respectively, is the impedance of the vacuum, is given in (2.3), both and have form: A 3 , L:=−ir×∇, Yℓ,m are spherical harmonics: and are the associated Legendre functions. Note that Xℓm fulfil the orthogonality relations where , and being proportional to the angular momentum operator, L satisfies L2Yℓm=ℓ(ℓ+1)Yℓm.
Expressing the electric and magnetic fields in terms of their components in the spherical coordinates, we have and , where Imposing the physical matching conditions at r=a1 and r=a2, we find that the tangential components of E and H are continuous along the boundaries, i.e. , , , and .
For TE modes, we can express these boundary conditions as A 4 where for all p,q=1,2, A 5 Note that these are, respectively, identical with (2.14) and (2.15), i.e. and LE=L. Therefore, as far as the study of the spectral singularities are concerned, we obtain similar results except that is now replaced by ℓ. As we see from (4.9), this does not influence the parameters of the system. It only changes the mode numbers associated with spectral singularities.
Similarly, for TM modes, we find the following set of boundary conditions. A 6 where, for all p,q=1,2, A 7 As we see the only difference between and Kpq is the appearance of the factor in the second row of . We have shown by explicit calculation that the presence of these extra factors does not affect the calculation of spectral singularities except for changing the value of the corresponding mode numbers.
↵4 For an experimental realization of the OSSs that we have examined, one may try to use the SHG of a diode-pumped Nd-YAG (continuous wave) laser at 532 nm wavelength in the plane-wave configuration. To achieve reasonably uniform gain, one probably needs to use multiple pumping. The details and a discussion of alternative pumping methods are beyond the scope of the present paper and the expertise of the authors.
- Received January 4, 2012.
- Accepted May 24, 2012.
- This journal is © 2012 The Royal Society