# Leaky Modes of Waveguides as a Classical Optics Analogy of Quantum Resonances

Authors: Sara Cruz y Cruz; Oscar Rosas-Ortiz
Journal: Advances in Mathematical Physics
 (2015)

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## Abstract

A classical optics waveguide structure is proposed to simulate resonances of short range one-dimensional potentials in quantum mechanics. The analogy is based on the well-known resemblance between the guided and radiation modes of a waveguide with the bound and scattering states of a quantum well. As resonances are scattering states that spend some time in the zone of influence of the scatterer, we associate them with the leaky modes of a waveguide, the latter characterized by suffering attenuation in the direction of propagation but increasing exponentially in the transverse directions. The resemblance is complete because resonances (leaky modes) can be interpreted as bound states (guided modes) with definite lifetime (longitudinal shift). As an immediate application we calculate the leaky modes (resonances) associated with a dielectric homogeneous slab (square well potential) and show that these modes are attenuated as they propagate.


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## Body

## 1. Introduction

In general, aresonance may be defined as the excitation of a system that results when one of its characteristic frequencies matches a particular value that is defined by either the boundary conditions, the external forces, or any other interaction or constraint applied to the system. The concept arises from the study of oscillating systems in classical mechanics and extends its applications to physical theories like electromagnetism, optics, acoustics, and quantum mechanics, among others [1]. In quantum and nuclear physics the resonances are associated with metastable states of a system which has sufficient energy to break up into two or more subsystems [2]. The whole range of scattering experiments provides a big number of examples in this matter [3, 4]. This last is because scattering includes the situation in which the impinging particle is “captured” for a while in the zone of influence of the scatterer, so that the projectile and the scatterer form a new unstable system (resonance state). The capturing occurs for specific energies of the projectile that are defined by the general properties of the scatterer. Eventually, the projectile is released and escapes from the interaction zone (decay process). In this model the “time of capture” corresponds to the lifetime of the decaying system that is formed of the scatterer and the projectile under the resonance condition. Collisions, in addition, are modeled as interactions localized in time and space. This implies that the involved potential vanishes rapidly enough in space, so that incoming and outgoing asymptotic states can be represented by wave packets in free motion. The problem is usually reduced to the analysis of one-dimensional effective potentials such that the main information is obtained from the transmission and reflection amplitudes of the scattering states; see, for example, [5]. In the case of one-dimensional square potential wells and barriers the resonances appear for specific values of the parameters that define the interaction. Indeed, for such parameters the resonances can be associated with the bell-shaped peaks of the corresponding transmission coefficient [6, 7]. The presence of resonances can be also stimulated either by shallowing a square well [8] or by adding to it a static electric field [9]. As resonances are special cases of scattering states, they are represented by irregular (not normalizable) vectors [10, 11] that satisfy the purely outgoing condition [12] (see also [1]). This last property of resonances is useful in constructing complex potentials that operate as optical devices with position-dependent complex refractive index [6, 13, 14].Remarkably, quantum wells and barriers can be made with high precision and compositional control by modern epitaxial growth techniques [15]. This has opened a wide window of experimental possibilities to explore various quantum phenomena in real devices and actual laboratory settings. For example, it has been shown that the transmission time of a wave packet that is tunnelling through a one-dimensional barrier does not depend on the barrier thickness [16]; a similar property is found in one-dimensional potential wells [17, 18]. This condition implies anomalously large group velocities of the wave packets that impinge the barrier (well) since the velocity of the packet’s peak must increase with the width across the interaction zone. Such a superluminal phenomenon has been observed using electromagnetic analogues for evanescent modes [19] and microwave pulses [20]; at the same time this result has stimulated the designing of high-speed devices based on the tunneling properties of semiconductors (see, e.g., Chapters 11 and 12 of [21]). On the other hand, as the scattering by quantum wells attenuates the outgoing wave packets only because of the multiple reflections at the well boundaries, it is expected that the resonance condition implies a maximum in the time spent by the projectile in traversing the zone of influence of the scatterer [6]. Recent theoretical research includes the case of a rectangular well that is embedded in an environment formed of a zero potential energy (flat potential) at the right and a parabolic potential at the left of the well [22–24]. Thus, the connection between time delay and “time of capture” associated with the scattering processes would be verified in the laboratory by using semiconductor materials.Another accessible laboratory tool to study quantum phenomena is provided by waveguide structures. The connection is based on the analogies between light waves and Schrödinger wave-state functions that have been studied since the early years of quantum physics [25]. In this approach the amplitude of an electromagnetic field is associated with the probability amplitude of a quantum state with two degrees of freedom while the propagation of such field through the waveguide corresponds to the time evolution of the quantum state. Such optical-quantum analogy is representative of a wider scheme that includes diverse connections between classical and quantum systems [26] and has been successfully applied in studying Anderson localization [27], coherent enhancement [28] and destruction of tunneling [29], coherent population transfer [30], and decay of metastable states coupled to semi-infinite, tight-binding lattices [31], among others. Of special interest for the purposes of this paper, nanoseconds delay-time measurements have been performed into the electromagnetic framework by using microwave setups of narrowed waveguides [32]. The relevance of this last result obeys the fact that the waveguide simulates a quantum potential barrier so that the measured electromagnetic delay-time is in correspondence with the quantum tunneling time. Thus, the waveguide structures represent an emergent and versatile arena to perform realistic experiments addressed to get deeper insights into the understanding of resonances in quantum physics.The aim of this paper is to get a classical optics analogy of the resonances associated with one-dimensional short range potentials in quantum physics. The centerpiece of our approach is the connection between the mathematical structure of the propagation of electromagnetic signals in waveguides and the dynamics of a time-dependent quantum state. In this form our interest is twofold: we want to connect the theoretical calculations of resonances with measurable properties of an electromagnetic wave that propagates in a waveguide and we would like to extend the application of the resonance mathematical techniques to the solving of problems associated with electromagnetic waveguides. A collateral result will be the connection between the resonance properties of electrons that are injected into heterostructures and the properties of the electromagnetic signals that propagate in optical waveguides. The paper is organized as follows. In Section2 we revisit the main properties of the resonance states associated with one-dimensional short range potentials. In particular, the relevance of the Fock-Breit-Wigner distribution in a scattering process is shown. When the transition amplitude from an initial scattering state to its time-evolved version is ruled by such a distribution, one immediately identifies energy resonances between the projectile and the scatterer. It is also shown that analytical continuation of the eigenvalue equation to a complex plane of energies is required to get an appropriate mathematical description of resonance states. In Section 3 we include some of the well-known generalities of the mode fields in waveguide structures and their connection with the Schrödinger equation of a system of two degrees of freedom. The case of electromagnetic propagation through a finite, dielectric homogeneous material and its association with a one-dimensional square well potential is considered in Section 3.1 as immediate application. Section 4 is devoted to the connection between resonance states and a singular form of modal field in waveguides; the latter is known asleaky mode and is characterized by suffering attenuation in the direction of propagation but increasing exponentially in the transverse directions. We apply the resonance approach of [6] in the calculation of the leaky modes associated with the dielectric homogeneous slab described in Section 3.1. As an example we provide thepropagation constant values (energy resonances) corresponding to the leaky modes supported by a slab of definite width and refractive index, and show that these modes are attenuated as they propagate. Section 5 includes the calculation of the longitudinal shifts for the leaky modes of Section 4; we show that the maxima of these shifts are in correspondence with the maxima of the transmission coefficient, a result that verifies the connection between times of capture and resonances in the scattering processes. Finally, Section 6 includes some of the main conclusions of the present work.


## 2. One-Dimensional Scattering States and Resonances

LetH be the Hamiltonian defined by a short range one-dimensional potential U(x). Assuming that the spectrum of H is formed of discrete and continuous eigenvalues, one can consider the following sets of state vectors: (1)discrete  eigenvaluesEk⟷ϕk,k∈ID⊆Z+ID=∑k∈IDϕkϕkHD=Span⁡⁡ϕkk∈ID,continuous  eigenvaluesE⟷ϕE,E∈IE⊆RIE=∫E∈IEdEϕEϕEHE=Span⁡⁡ψEE∈IE, where ID and IE are, respectively, the identity operator in HD and HE. Consistently, the spectrum and Hilbert space of H are σ(H)={Ek}k∈ID∪{E}E∈IE and H=HD⊕HE, respectively. As usual, the discrete and continuous eigenvectors (1) are orthonormal in their respective subspace according to the rules (2)ϕj∣ϕk=δjk,ϕE∣ϕE′=δE-E′. Hereafter we pay detailed attention to the scattering states (i.e., vectors in HE). The description of bound states (i.e., vectors in HD) is straightforward by using the well-known relationship ∫dE↔∑k. The reason is that, as we have said in the introduction, resonance states arise quite naturally in the scattering processes.Any scattering state|ψ〉∈HE can be expressed in the basis of continuous eigenvectors (3)ψ=IEψ=∫E∈IEdECEϕE,CE=ϕE∣ψ, and is such that (4)ψ2=ψ∣ψ=∫E∈IEdECE2. In x-representation the above expressions read as (5)ψx=∫E∈IEdECEϕEx,CE=∫Rdxϕ¯Exψx,(6)ψ2=∫Rdxψx2=∫E∈IEdECE2, with z¯ standing for the complex conjugate of z∈C. The above expressions allow writing the energy distribution ω(E) as follows: (7)ωE=dWdE=CE2. Let (3), equivalently (5), be the initial state of a stationary system. The transition amplitude T(t≥0) from |ψ(t=0)〉=|ψ0〉 to |ψ(t)〉=|ψt〉 is given by the inner product (8)Tt≥0=ψ0∣ψt=∫Rdxψ¯0xψtx=∫E∈IEdEωEe-iEt/ħ. It is clear that T can be investigated in terms of spatial coordinates x or as a function of the energy distribution (7). In this work we will assume that ω(E) is given by the following expression: (9)ωE=Γ/22E-E0+iΓ/2E-E0-iΓ/2=Γ/22E-E02+Γ/22, where E0∈IE is the energy of the initial state |ψ0〉 and Γ≥0 is a parameter having units of energy. Note that the bell-shaped function (9) is centered at E=E0, for which ω(E0)=1, and has a half-width at half-maximum equal to Γ/2. In addition, ω(E) is a meromorphic function that has two poles E±=E0±iΓ/2. This function is known as either Cauchy (mathematics), Lorentz (statistical physics), or Fock-Breit-Wigner (FBW) (nuclear and particle physics) distribution. Using (7) we can write the Fourier coefficient C(E) in the expansion (3) as follows: (10)CE=Γ/2E-E0+iΓ/2.After the analytic continuation of IE⊆R to the complex E-plane one can introduce (9) into (8) to arrive, up to a global constant factor, at the expression (11)Tt≥0=Γ2e-iɛ0t/ħ=Γ2e-iE0t/ħe-Γt/2ħ,ɛ0≔E0-iΓ2. This last result has the form of a transient oscillation [1] and means that the transition from |ψ0〉 to |ψt〉 is an exponential decreasing function of time whenever C(E) is given by (10). That is, the initial state |ψ0〉 decays according to the time-dependent probability (12)Tt≥02=Γ22e-Γt/ħ. As we can see, the width Γ of the distribution (9) represents an indirect measure of the lifetime of |ψ0〉 because at time τ:=ħ/Γ the probability that this state has not yet decayed is reduced approximately in 36%, that is, Γ2/4→Γ2/(4e). It is clear that Γ and τ are correlated; the smaller the value of Γ the larger the lifetime τ. In general, one says that there is a resonance E0 of width Γ when either the energy distribution of the system at time t≥0 is given by the FBW function (9) or the Fourier coefficients C(E) of the expansion (3) are given by (10).We would like to emphasize that the dependence ofω, C, and T on the complex number ɛ0=E0-iΓ/2, as this has been expressed in (9)–(12), is not merely aesthetic; this corresponds to the formulation developed by Gamow, Fock, Breit, and Wigner in the late 1920s and along the 1930 decade (see details in [1]). It is due to Siegert [12] that a resonance is introduced as a solution uɛ of the Schrödinger equation associated with the complex eigenvalue ɛ=E-iΓ/2 and satisfying the purely outgoing condition [6]: (13)limx→±∞⁡β=∓ik, where k2=2mɛ/ħ2∈C and (14)β≔-ddxln⁡uɛ. It can be shown that the above conditions lead automatically to the FBW distribution (9) with k a number in the fourth quadrant of the complex plane C; see [1]. In turn, the distribution of the complex points ɛ1/2=ħk/2m characterizes a Riemman surface of two sheets, each one cutting along the positive real axis. These complex numbers define directly the behavior of the propagator (12). For instance, consider a very narrow distribution ω(E), that is, Γ≪1 (the point ɛ∈C is close to the positive real axis). As Γ defines the vicinity E∈(E0-Γ/2,E0+Γ/2), we see that “large lifetimes” τ=ħ/Γ means narrow widths Γ, so that the energy E of the system at time t≥0 is very close to the initial energy E0. In the extremal case Γ→0, the distribution ω(E) is as narrow and singular as δ(E-E0). That is, the related lifetime τ is large enough (τ→+∞) to consider the initial vector |ψ0〉 a nondecaying (stable) state. In this context, bound states are considered as decaying states with infinitely large lifetimes and vice versa, unstable (decaying) states correspond to bound states with a definite lifetime.To get more insights into the complex eigenvalueɛ0 let us consider the Schrödinger equation (15)Hψx;t=iħddtψx;t. Assuming separation of variables ψ(x;t)=φ(x)θ(t), with θ(t)=e-iEt/ħ and E∈IE the separation constant, the probability density does not depend on time |ψ(x;t)|2=|φ(x)|2. Now, let us make the analytic continuation of the eigenvalue equation Hφ(x)=Eφ(x) in order to include complex eigenvalues ɛ=E-iΓ/2, that is, Huɛ=ɛuɛ. In this case we have ψ(x;t)=uɛ(x)e-iɛt/ħ, and the probability density is an exponential decreasing function of time |ψ(x;t)|2=|uɛ(x)|2e-Γt/ħ. Clearly, the spatial part uɛ(x) of the wave-function ψ(x;t) is no longer a square-integrable function because this belongs to the complex eigenvalue ɛ and the Hamiltonian H is still Hermitian. Indeed, it can be proved that uɛ(x) diverges exponentially as |x|→+∞. Thus, the density |ψ(x;t)|2 increases exponentially for either large |x| or large negative values of t. The usual form to avoid some of the complications connected with the limit t→-∞ is to consider the long lifetime limit Γ→0; see, for example, [33]. Therefore, we consider the condition (16)Γ/2ΔE≪1. This last means that the level width Γ must be much smaller than the level spacing ΔE in such a way that closer resonances must imply narrower widths (longer lifetimes). In general, the main difficulty is precisely to find the adequate E and Γ. However, it has been shown [6] that for one-dimensional stationary short range potentials the superposition of a denumerable set of FBW distributions (each one centered at each resonance En, n=1,2,…) entails an approximation of the transmission coefficient T such that the larger the number N of resonances involved, the higher the precision of the approximation:(17)T≈ωNE=∑n=1NωE,En;ωE,En=Γn/22E-En2+Γn/22.


## 3. Mode Fields in Waveguide Structures

Consider the Helmholtz equation(18)∂2∂x2Ex,z+∂2∂z2Ex,z+k02n2xEx,z=0, with k0=w/c the wave number in vacuum. Equation (18) can be achieved from the Maxwell equations for transversal electric fields E→ in presence of inhomogeneous dielectric materials, neglecting the magnetic polarizability and the dispersive properties of the medium. Indeed, (18) corresponds to an electric wave propagating along the positive z-direction and polarized in the y-direction, assuming that the refractive index n depends only on the x-coordinate. In the paraxial regime we use the ansatz (19)Ex,z=φxe-ik0γ-n0z, to transform (18) into the linear second-order differential equation (20)-12k02n0d2dx2-nxφx=ɛφx,ɛ=γ-n0, known as the paraxial Helmholtz equation. In (19)-(20) the number n0 is a reference refractive index that may be taken as the maximum of n(x), and we have assumed that the weakly guiding condition (Δn=|n-n0|≪1) holds. In this approach the parameter ɛ, known as the propagation constant, is the value of the z-component of the generalized linear momentum [34] and defines the slope of the light beam as follows: (21)ɛ=-pz=-nxcos⁡θx.In general, modal fields associated with open waveguides are classified into guided (trapped) modes and radiation modes, the latter propagating outside the core [35–38]. The guided modes are bounded fields that correspond to real values of the propagation constant fulfilling -n0≤ɛ<-1. They are perfectly guided through the waveguide as they suffer no attenuation along the optical axis and decay exponentially in the transverse direction. Thus, as guided modes are trapped into the core of the waveguide they add no energy flux into the infinite surrounding clad. In turn, propagating radiation modes correspond to real propagation constants fulfilling -1≤ɛ<0, so that they are oscillatory fields in the transverse as well as in the longitudinal directions [35]. They appear as a consequence of the infinite extension of the clad cross section. Guided and radiation modes constitute a complete set of modal fields in the sense that any physical solution to the paraxial Helmholtz equation can be expressed as a linear superposition of a finite number of guided modes and a continuum of radiation modes.At this stage it is important to stress the resemblance of the electric field expression (19) with the solutions ψ(x;t)=φ(x)e-iEt/ħ of the Schrödinger equation (15). This allows the identification (22)k0-1⟷ħ,z⟷t,ɛ=γ-n0⟷E. In adittion, (20) would correspond to the eigenvalue equation Hφ=Eφ, provided the following additional identification holds: (23)H=-k0-22n0d2dx2-nx,n0⟷m,-nx⟷Ux. The identification (22)-(23) is well known in the literature; see, for example, [34]. This allows to construct the classical optics analogy of diverse quantum phenomena and vice versa, the quantum analogy of classical optical phenomena [26, 34]. The analogy includes the sets of vectors introduced in (1) because bound states correspond to “trapped” waves that have no chance of escaping from the zone of influence of the scatterer (as we have seen in the previous section, these states can be interpreted as decaying states with infinitely large lifetime). Thus, quantum bound states correspond to guided electromagnetic modes. Particles in scattering states, on the other hand, can be temporally trapped by the scatterer in such a form that their presence in the zone of interaction decreases in time. In this form, scattering states correspond to radiation modes. The orthonormalization properties of guided and radiation modal fields can be stated in a form similar to that of the quantum mechanical bound and scattering states (see, e.g., [35, 37]). Hence, the total radiated power can be expressed as the sum of two terms: the first one associated with the power that propagates inside the core, given by a finite sum containing the contribution of guided modes, and a second term corresponding to the power radiated from the core, expressed as an integral over all radiation modes. In this form, denoting by Ak and A(ɛ) the guided and the radiation mode amplitudes, respectively, the total power of the radiated field in the waveguide axis direction is given by [36] (24)Prad=∑kAk2+∫ɛ∈IɛdɛAɛ2. On the other hand, as we have seen, resonances are scattering states of complex eigenenergy that spend definite intervals of time in the interaction zone. So resonances are not connected to radiation modes because these last do not belong to complex eigenvalues. Next we will take full advantage of the analogy indicated above to get optical models for the resonances discussed in Section 2.


### 3.1. Wave Propagation through a Dielectric Homogeneous Slab

As an immediate application let us analyze the simplest case of electromagnetic propagation through a finite, dielectric homogeneous material. It is convenient to rewrite the eigenvalue equation (20) as follows: (25)-k0-22n0d2dx2+1-nxφ=ɛ+1φ. Considering a combination of media distributed along the x-axis such that there is vacuum in (-∞,-a)∪(a,+∞) and a medium of constant refractive index n=U0>1 in x∈[-a,a], (25) is in correspondence with the eigenvalue equation defined by a linear square well of depth V0=|1-U0| and width 2a. The solutions to this equation are well known and can be found elsewhere, though the analysis of resonances and the resolution of the transmission coefficient in terms of the FBW distribution (see (17)) can be consulted in [6]. Hereafter we will label the regions of the media (vacuum, medium, vacuum) from left to right as I, II, and III.


## 3.1. Wave Propagation through a Dielectric Homogeneous Slab

As an immediate application let us analyze the simplest case of electromagnetic propagation through a finite, dielectric homogeneous material. It is convenient to rewrite the eigenvalue equation (20) as follows: (25)-k0-22n0d2dx2+1-nxφ=ɛ+1φ. Considering a combination of media distributed along the x-axis such that there is vacuum in (-∞,-a)∪(a,+∞) and a medium of constant refractive index n=U0>1 in x∈[-a,a], (25) is in correspondence with the eigenvalue equation defined by a linear square well of depth V0=|1-U0| and width 2a. The solutions to this equation are well known and can be found elsewhere, though the analysis of resonances and the resolution of the transmission coefficient in terms of the FBW distribution (see (17)) can be consulted in [6]. Hereafter we will label the regions of the media (vacuum, medium, vacuum) from left to right as I, II, and III.


## 4. Leaky Modes and Resonances

Besides the guided and radiation modes discussed in the previous section, it is well known the existence of solutions to the Helmholtz equation with complex propagation constants that have an “unusual behavior”: they increase exponentially in the transverse direction and suffer attenuation in the longitudinal one [35]. These solutions are called leaky modes and have attracted much attention over the time. The leaky modes do not belong to the set of guided and radiation modes of infinite transverse waveguides, though they constitute a discrete set of modes that can be used to approximate the continuous mode contribution to the radiation field, in regions close to the core and far from the source, in order to avoid integration overall radiation modes [36–40]. Yet, leaky modes have properties that are very similar to the ones of guided modes, but the former modes loss energy as they propagate along the optical axis [37]. In slab waveguides this leakage is due to refraction at the waveguide core-clad boundaries (refracting leaky modes [36]). In waveguides with curved cross section the leakage can be also produced by the partial reflection at the boundaries due only to the curvature of the cross section (tunneling leaky modes) [35, 36]. It can be shown that the leakage is slower in the tunneling modes compared to the refractive modes [35]. In any case, these modes behave much like guided modes as they are able to propagate large distances inside the guide before their power loss started to be significant. Different methods have been applied to determine the leaky modes of planar [37, 41] as well as cylindric [35, 39] waveguides involving isotropic and anisotropic dielectrics [42]. These techniques include numerical methods as mode-matching [43], finite differences and finite element [38, 42, 44], approximate methods as WKB [45], transfer matrix [41] and differential transfer matrix methods [40, 46]. In contrast to the diversity of mathematical techniques to determine the propagation constants of leaky modes there is still a conceptual discussion concerning them, the exponential growing in the transversal direction of these nearly guided modes make them appear as nonphysical solutions to the Helmholtz equation. Yet, this behavior is required if the energy flux must be preserved: as the flux is damped in the longitudinal direction, there must be an increasing flux in the transverse direction [37].The problem of finding leaky modes is mathematically equivalent to determine the resonant states in quantum mechanics for a particle in a short range interaction potential. This is convenient because we may apply different methods that have been addressed to obtain the resonance energies and the corresponding wave functions in order to determine the complex propagation constants and the modal fields. To this end, let us regard the square well potential analogy indicated in Section3.1 with a complex propagation constant, ɛ=ɛR-iΓ/2. The corresponding complex wave number k=kR+ikI is related to ɛ through(26)ɛR=kR2-kI22k02-1,-Γ2=kRkIk02.The energy density flux in the transverse direction is not null because kR≠0 (see [6]). A wave coming from region III enters into resonance with the optical medium and is thus trapped inside the core (region II); then it propagates and travels a finite distance along the optical axis. After a while, the wave is finally emitted into the clad. The result is a wave propagating to the left in region I and another one propagating to the right in region III. The correct sign for kR is thus positive and the whole process obeys the pure outgoing condition. The expression for the electric energy density fulfills(27)limx→±∞⁡ρe∝e-k0Γzφx2,meaning that the power decreases exponentially as z grows whenever Γ>0 and kI<0. The optical-quantum analogy requires also a purely outgoing wave φ(x) (see Section 2) so the amplitudes of the external electric fields increase exponentially as x→±∞. Leaky modes then correspond to wave numbers k=kR+ikI in the fourth quadrant of the complex plane. The factor k0-1/Γ can be interpreted as the mean distance traveled by the beam, along the optical axis, before its intensity decays by 1/e of its intensity at a focus. In this context Γ represents a measure of the transient confinement of the field into the core. In the limit Γ→0 we will have a quasistationary mode propagating inside the slab in a very similar way as a guided mode. In this limit, it is possible to establish an analytic approach to calculate the propagation constant. Bearing this in mind, following (16), we may write(28)Γ/2ΔɛR≪1,where ΔɛR is the separation between two consecutive resonances. To get the position ɛR and the width Γ of the resonances we follow the approximations reported in [6]. After some calculations one arrives at the expressions(29)ɛR≈12k02U0mπ2a2-U0,Γ2≈1k0aU02ɛR+1,with m an integer number fulfilling(30)2U0U0-1<mπ2k0a<2U02.Thus, for each combination of the parameters a,U0,k0, there is a finite number of resonances given by (29). Table 1 shows the propagation constants ɛ corresponding to the 17 leaky modes supported by a slab waveguide of refractive index U0=1.5 and width k0a=30. The behavior of the real part of the field amplitude of these modes, as they propagate in the longitudinal direction through the waveguide, is depicted in Figure 1 for m=24 (left), m=32 (center), and m=40 (right). Observe that the modes with smaller values of m attenuate slower compared to those with larger values of m.Table 1
Propagation constant valuesε corresponding to the 17 leaky modes supported by a slab of width k0a=30 and constant refractive index U0=1.5.
k
0
a
=
30, U0=1.5
m
ε
=
ε
R
-
i
Γ
2
Γ
X
X
24
-
0.973621
-
i
0.0051042
25
-
0.928842
-
i
0.0083833
26
-
0.882236
-
i
0.0107847
27
-
0.833802
-
i
0.0128120
28
-
0.783540
-
i
0.0146215
29
-
0.731450
-
i
0.0162860
30
-
0.677533
-
i
0.0178462
31
-
0.621788
-
i
0.0193273
32
-
0.564215
-
i
0.0207462
33
-
0.504815
-
i
0.0221150
34
-
0.443587
-
i
0.0234424
35
-
0.380531
-
i
0.0247350
36
-
0.315647
-
i
0.0259981
37
-
0.248936
-
i
0.0272358
38
-
0.180397
-
i
0.0284514
39
-
0.110031
-
i
0.0296476
40
-
0.037836
-
i
0.0308267Figure 1
Propagation of resonances inside a slab waveguide of widthk0a=30 and constant refractive index n=U0=1.5. The slab supports 17 leaky modes (24≤m≤40) defined by (29). The figure shows the propagation in the axial direction (from the bottom to the top in each slab) of the real part of the leaky modes field amplitudes for m=24 (left), m=32 (center), and m=40 (right). Note that these are attenuated as the mode propagates. The leakage is faster for larger values of m.


## 5. Longitudinal Shifts

Let us determine the longitudinal shift of a wave packet under scattering by an optical medium. This will provide us some insight into the mean distance traveled by the leaky mode in the waveguide before the longitudinal power is completely lost. This problem is equivalent to evaluating the reflection and transmission phase times for a particle in a rectangular well potential [16, 17, 47]. Consider a wave-packet scattering solution for the external electric field(31)EIx,z=∫0κdkfkeikx-k0ɛkz+∫0κdkfkrkei-kx-ɛkk0z-2ka+ϕk,EIIIx,z=∫0κdkfktkeikx-ɛkk0z-2ka+ϕk+π/2,where f(k) is the Fourier coefficient, κ is defined by ɛ(κ)=0, r(k) and t(k) are the reflexion and transmission amplitudes, respectively, and(32)ϕk=-arctan⁡2kqcos⁡2qak2+q2sin⁡2qa,q2=U0k2+2k02U0-1.Applying the stationary phase condition [16, 23, 24] to the incident and transmitted wave packets, one has(33)∂∂kkx-k22k0z+k0z=0,∂∂kkx-2ka-k22k0z+k0z+ϕk+π2=0.So that the equations of motion for the centers of the corresponding Fourier components are given by(34)x=kk0z,x=2a+kk0z+∂ϕ∂k.The point zin at which an incident plane wave of wave number k would reach the left wall of the optical medium is then zin=-k0/ka. In the same way the point zt at which the reflected or transmitted wave leaves the optical medium is(35)zt=k0k-a+∂ϕ∂k.Then the longitudinal shift of the reflected or transmitted wave is readily written as(36)δz=zt-zin=k0k∂ϕ∂k.Figure 2 shows the longitudinal shift of a Fourier component under reflection or transmission as a function of ɛ for (a) k0a=30 and (b) k0a=5×104. It is worthwhile pointing out that the peaks of this shift coincide with the peaks of the corresponding transmission coefficient as shown in Figure 3. This implies that the electromagnetic modes having maximum transmission probabilities and thus corresponding to the resonant (leaky) modes travel a maximum longitudinal distance in the core before they are finally transmitted to the infinite clad. Figure 4 shows the longitudinal shift as a function of the width k0a for the propagation constant ɛ=-0.995 and U0=1.5. We can appreciate that the transmission shift δz takes negative values; these have been already predicted for both rectangular barriers and wells in the quantum approach [17, 47]. The analogy between the Schrödinger and the paraxial Helmholtz equations suggests that this property may be used to measure the negative phase time in the scattering of particles by a potential well (compare with [18]).Figure 2
Longitudinal shift as a function of the propagation constantɛ=-pz for a dielectric slab of width k0a equal to (a) 30 and (b) 5×104. In both cases U0=1.5.
(a)
(b)Figure 3
Longitudinal shift (continuous line) and transmission coefficient (dotted line) of an electric wave propagating in a dielectric slab of widthk0a=30 and constant refractive index U0=1.5, both as a function of the propagation constant ɛ. Observe that the maxima of both curves coincide.Figure 4
Longitudinal shift as a function of the widthk0a of a dielectric slab with constant refractive index U0=1.5. Here ɛ=-0.995.


## 6. Conclusions

The classical optics analogy of quantum systems is based on the relationship between the Helmholtz equation and the two degrees of freedom Schrödinger equation. Although such analogy is mathematical, the optical solutions are useful in simulating the quantum ones for diverse cases. For instance, it is well known that the guided and radiation modes of a waveguide structure can be put in correspondence with the bound and scattering states of a one-dimensional short range potential in quantum mechanics. However, the association of leaky modes with their quantum counterpart, as well as the identification of the optical analogue of a quantum resonance, is rarely discussed in the literature on the matter. One of the reasons would be that in both cases the calculation of the eigenvalues and wave solutions is not as immediate as in the scattering (radiation) or bound (guided) states (modes). In this work we have presented a form to connect these two kinds of wave solutions: a leaky mode is in correspondence with a resonance state. The former is as close to a guided mode as a resonance is close to a bound state. That is, a leaky mode (resonance state) is a guided mode (bound state) for which the longitudinal shift (lifetime) is definite.



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*Source: 281472-2015-08-30.xml*