Abstract
The Born approximation (Born 1926 Z.Phys.38.802) is a fundamental result in physics, it allows the calculation of weak scattering via the Fourier transform of the scattering potential. As was done by previous authors (Ge et al 2014 New J. Phys. 16 113048) the Born approximation is extended by including in the formula the resonant-states (RSs) of the scatterer. However in this study unlike previous studies the included eigen-modes are correctly normalised with dramatic positive consequences for the accuracy of the method. The normalisation of the RSs used in the previous RSE Born approximation or resonant-state-expansion Born approximation made in Ge et al ( A 93 023835). In the case of effectively one-dimensional systems I find an RSE Born approximation alternative to the scattering matrix method.
I. INTRODUCTION
Fundamental to scattering theory, the Born approximation consists of taking the incident field in place of the total field as the driving field at each point inside the scattering potential, it was first discovered by Max Born and presented in Ref. [1] . The Born approximation gave an expression for the differential scattering cross section in terms of the Fourier transform of the scattering potential. The Born approximation is only valid for weak scatterers as we will see in the numerical demonstrations.
I. INTRODUCTION
In this paper I provide an extension to the Born approximation which allows an arbitrary number of resonant states (RSs) to be taken into account. I have named this extension to the Born approximation the Resonantstate-expansion correction to the Born approximation or the RSE Born approximation. An almost identical approach is already available in the literature [2] however its derivation differed by including an unstable normalisation formula for the RS eigen-modes of the system which was then subsequently used to expand Born's approximation incorrectly. The normalisation derived in Ref. [15] and used in the previous RSE Born approximation made in Ref. [2] has been shown to be numerically unstable in Ref. [10] and shown to be unstable using analytics in Appendix C. Furthermore the numerical study made in Ref. [2] only included a single RS in the expansion of the Born approximation, most likely to avoid divergence caused by their incorrect normalisation of the RSs.
I. INTRODUCTION
Recently there has been developed [3, 8, 9 ] a rigorous perturbation theory called resonant-state expansion (RSE) which was then applied to one-dimensional (1D), 2D and 3D systems [4-7, 11, 12] which only calculates the modes and makes no use of them. The RSE accurately and efficiently calculates RSs of an arbitrary system in terms of an expansion of RSs of a simpler, unperturbed one. RSs are normalised correctly to appear in spectral Green's functions (GFs) via the flux volume normalisation [7] and hence the RSE Born approximation. In the limit where an infinite number of these resonances are included in the RSE Born approximation we will observe convergence of the method towards the exact solutions. That the RSE can reproduce both the correctly normalised RS fields as well as frequencies was demonstrated in Ref. [4] with the convergence and extrapolation algorithm which I contributed to that paper.
I. INTRODUCTION
Interestingly the resonant-state-expansion is a near identical translation to Electrodynamics of a much earlier theory from Quantum Mechanics by More, Gerjuoy, Bang, Gareev, Gizzatkulov and Goncharov Ref. [8, 9] . The only difference between the two approaches is the choice of RS normalisation method. I am able to show in this manuscript that the general normalisation of resonant-states which I derived in Ref. [7] is the most numerically stable available normalisation method. The general normalisation which I derived in Ref. [7] is based on a prototype normalisation which appeared in Ref. [3] .
I. INTRODUCTION
The concept of RSs was first conceived and used by Gamow in 1928 in order to describe mathematically the process of radioactive decay, specifically the escape from the nuclear potential of an alpha-particle by tunnelling. Mathematically this corresponded to solving Schrödinger's equation for outgoing boundary conditions (BCs). These states have complex frequency ω with negative imaginary part meaning their time dependence exp(−iωt) decays exponentially, thus giving an explanation for the exponential decay law of nuclear physics. The consequence of this exponential decay with time is that the further from the decaying system at a given instant of time the greater the wave amplitude. An intuitive way of understanding this divergence of wave amplitude with distance is to notice that waves that are further away have left the system at an earlier time when less of the particle probability density had leaked out. There already exists numerical techniques for finding eigenmodes such as finite element method (FEM) and finite difference in time domain (FDTD) method to calculate resonances in open cavities. However determining the effect of perturbations which break the symmetry presents a significant challenge as these popular computational techniques need large computational resources to model high quality modes. Also these methods generate spurious solutions which would damage the accuracy of the RSE Born approximation if included in the basis.
I. INTRODUCTION
The paper is organized as follows, Sec. II outlines the derivation of the RSE Born approximation, Sec. III discusses normalisations of RSs by other authors, Sec. IV outlines the application of the RSE Born approximation to planar slabs, Sec. V gives the numerical validation of the new method along with a comparison of the alternative RSE approaches.
II. DERIVATION OF THE RSE BORN APPROXIMATION
I will in the following section re-derive the method for calculating the full GF of an open electrodynamic system in the same way as Ref. [2] however unlike previous authors I use the numerically stable normalisation of RSs which I derived in Ref. [7, 12] . These methods are required to calculate transmission and scattering crosssection from the dispersive RSE perturbation theory with mathematical rigour and accuracy.
II. DERIVATION OF THE RSE BORN APPROXIMATION
For an electrodynamic system with local frequency dependent dielectric permittivity tensorε k (r) and permeability µ = 1, where r is the three-dimensional spatial position, Maxwell's wave equation for the electric E(r)-field with a current source J(r) oscillating at frequency k, which can be real or complex, is
II. DERIVATION OF THE RSE BORN APPROXIMATION
The time-dependent part of the field is given by exp(−iωt) with the complex eigen-frequency ω = ck, where c is the speed of light in vacuum. The Green's function (GF) of an open electromagnetic system is a tensorĜ k which satisfies Maxwell's wave equation Eq. (1) with a delta function source term,
II. DERIVATION OF THE RSE BORN APPROXIMATION
where1 is the unit tensor. Physically, the GF describes the response of the system to a point current with frequency ω, i.e. an oscillating dipole. The importance ofĜ k comes from the fact we can see from Eqs. (2) that Eqs. (1) can be solved for E(r) by convolution ofĜ k with the current source J(r ′ ),
II. DERIVATION OF THE RSE BORN APPROXIMATION
Inside the system we can use the RSE to calculate the GF. In Appendix A I derive for dispersive systems (for which I have recently developed a dispersive RSE perturbation theory [11, 12] ) a convenient form of the spectral GF, valid inside the scatterer only,
II. DERIVATION OF THE RSE BORN APPROXIMATION
The E n are RSs of the open optical system and are defined as the eigen-solutions of Maxwell's wave equation,
II. DERIVATION OF THE RSE BORN APPROXIMATION
satisfying the outgoing wave BCs. I have also taken the resonator to be embedded in free space (ε = 1) without loss of generality. Here, k n is the wave-vector eigen-value of the RS numbered by the index n, and E n (r) is its electric field eigen-function. The RSs which are solutions of Eq. (5) which are either stationary or decaying in time.
II. DERIVATION OF THE RSE BORN APPROXIMATION
Modes appearing in Eq. (4) are normalized [7, 12] according to the flux-volume normalisation
II. DERIVATION OF THE RSE BORN APPROXIMATION
where the first integral is taken over an arbitrary simply connected volume V enclosing the inhomogeneity of the system and the center of the spherical coordinates used, and the second integral is taken over its surface S V . This normalization is required [7] for the validity of the spectral representation Eq. (4). Numerically Eq. (6) has been validated by its use in RSE perturbation theory [4-7, 11, 12] . A discussion of the dispersive RSE for nano-particles is given in Appendix B.
II. DERIVATION OF THE RSE BORN APPROXIMATION
The generalisation of my Eq. (6) to k n = 0 modes is attributable solely to E. A. Muljarov in Ref. [7] (I derived the normalisation proof for Ref. [7] without k = 0 modes), however that part of the proof of the normalisation can only be further generalised to dispersive systems using the spectral GF Eq. (4) derived in Appendix A. The required derivation is identical except that it makes use of the rigorously derived spectral GF Eq. (4) instead of the identical GF derived in a less mathematically rigorous way for non-dispersive systems. This last step is vital for the accuracy of the method. Further I note that just as I explained in Ref. [12] ε k must be a symmetric matrix or a scalar in order to calculate the dispersion factor as shown.
II. DERIVATION OF THE RSE BORN APPROXIMATION
Various schemes exist to evaluate the surface integral limit in Eq. (6) such as analytic methods in Ref. [3, 7, 10] or numerically extending the surface into a nonreflecting, absorbing, perfectly matched layer where it vanishes.
II. DERIVATION OF THE RSE BORN APPROXIMATION
The derivation of the RSE Born approximation by Ge et al. [2] has been made using the normalization introduced by Leung et al. [15] the limit of infinite volume V is taken:
II. DERIVATION OF THE RSE BORN APPROXIMATION
It was numerically found [13] that the surface term was leading to a stable value of the integral for the relatively small volumes available in 2D finite difference in time domain (FDTD) calculations. However, it was discovered at the time that this was not the case for low-Q modes. It was wrongly shown by Muljarov et al [10] that Eq. (7) is actually diverging in the limit V → ∞, and therefore the expansion of the Born approximation in [2] and the normalization Eq. (7) are incorrect. In Appendix C I provided a mathematically rigorous disproof of some of E. A. Muljarov's points and make some correct points about the unsuitability of Eq. (7) for the RSE perturbation theory myself. Hence although being a cornerstone of the scattering theory of open systems the correct expansion of the Born approximation in terms of RSs to the exact solution was not previously available.
II. DERIVATION OF THE RSE BORN APPROXIMATION
Analogously to Ref. [2] the derivation of the RSE Born approximation of Ge et al. [2] is made but in this case using my correct normalisation formula for modes.
II. DERIVATION OF THE RSE BORN APPROXIMATION
That the E n (r) and k n can be calculated accurately by the RSE perturbation theory and normalised correctly by Eq. (6) makes possible the RSE Born approximation.
II. DERIVATION OF THE RSE BORN APPROXIMATION
The free space GFĜ f s k is now introduced
II. DERIVATION OF THE RSE BORN APPROXIMATION
which has the solution,
II. DERIVATION OF THE RSE BORN APPROXIMATION
The systems associated withĜ k andĜ f s k are related by the Dyson Equations perturbing back and forth with
II. DERIVATION OF THE RSE BORN APPROXIMATION
Combining Eq. (10) and Eq. (11) it is obtained as in Ref.
II. DERIVATION OF THE RSE BORN APPROXIMATION
[2]
II. DERIVATION OF THE RSE BORN APPROXIMATION
In order to improve the numerical performance further I make a final few steps as in the original Born approximation [1] , I define unit vectorr such that r = rr and k s = kr. Then for r >> r ′ ,
II. DERIVATION OF THE RSE BORN APPROXIMATION
Therefore substituting Eq. (4) and Eq. (9) in to Eq. (12) and using Eq. (13) because both r, r ′′ are far from the scatterer we arrive at the RSE Born approximation
II. DERIVATION OF THE RSE BORN APPROXIMATION
. (14) or using Eq. (A1) instead
II. DERIVATION OF THE RSE BORN APPROXIMATION
The vector A n is defined as a Fourier transform of the RSs,
II. DERIVATION OF THE RSE BORN APPROXIMATION
I note that the fast Fourier transform method is available. Furthermore I note that for the inverse scattering problem at resonance the inverse Fourier transformation is also available. The first two terms in Eq. (15) correspond to the standard Born approximation, the final summation term corresponds to the RSE correction to the Born approximation. A simple corollary of this theory is as follows, we can see from the arguments just stated that from Eq.(10) if r ′′ is inside the resonator and r >> r ′′ then
II. DERIVATION OF THE RSE BORN APPROXIMATION
or using Eq. (A1) instead
II. DERIVATION OF THE RSE BORN APPROXIMATION
similarly from Eq. (11) if r is inside the resonator and r ′′ >> r then
II. DERIVATION OF THE RSE BORN APPROXIMATION
or using Eq. (A1) instead
II. DERIVATION OF THE RSE BORN APPROXIMATION
other permutations are possible.
III. OTHER NORMALISATIONS A. Normalisation by Sauvan and co-workers
The rigorously derived normalisation of Sauvan and co-workers that they gave in Ref. [18] as
III. OTHER NORMALISATIONS A. Normalisation by Sauvan and co-workers
requires that the integral V be continued into a perfectly matched layer where it is attenuated to zero, thus eliminating the need for surface terms in the normalisation. As such it is most suitable for FEM and FDTD calculations. Further I note that just as I explained in Ref. [10] ε k (r) must be a symmetric matrix or a scalar in order to calculate the dispersion factor as shown.
III. OTHER NORMALISATIONS A. Normalisation by Sauvan and co-workers
I generate this normalisation by combining the RSE normalisation for H n and E n , I note that this alternative approach to deriving Sauvan's normalisation was discussed with E. A. Muljarov at some point but without discussing k n = 0 modes. I also note that k n = 0 modes have only H field or E field component by Maxwell's equations because they are curl free modes. k n = 0 are by definition modes which satisfy the condition of being curl free. These two points explain why the addition of k n = 0 modes to Sauvan and co-worker's normalisation takes the form it does. Actually the RSE normalisation for H n modes was first shown to me in an email attachment, by E. A. Muljarov several years ago but without any derivation and without k n = 0 modes or differential dispersion factor included.
III. OTHER NORMALISATIONS A. Normalisation by Sauvan and co-workers
The rigorous derivation of the relationship between normalised E-field and normalised H-field can be found in appendix D of my PhD thesis [20] .
III. OTHER NORMALISATIONS A. Normalisation by Sauvan and co-workers
Clearly as the perturbation is increased there is a critical perturbation strength at which the RSE becomes less efficient than FDTD and FEM and beyond this point one should use the RSE Born approximation with the normalisation of Ref. [18] and FDTD or FEM.
B. Radiation mode normalisation
I have recently written a paper on the RSE Born approximation for waveguides with dispersion [12] . I found that such modes for cylindrical/effectively-2D waveguides can be normalised by reducing Maxwell's equation to effectively 2D and replacing the operation ∇×∇× with a suitable linear operator L invariant along the length of the waveguide. A similar approach is found in Ref. [19] and further comparison of the two methods is required.
IV. APPLICATION TO PLANAR SYSTEMS
In this section we discuss the application of the RSE Born approximation to exactly solvable 1D scattering problems in electrodynamics. This is in order to prove the converges of the new method to the exact solutions available for 1D problems in Sec. V. The dielectric profile is described by a scalar frequency independent dielectric profile, i.e.ε k (z) =1ε(z), ∆ε k (z) =1∆ε(z). As unperturbed system we use a homogeneous planar slab of half width a, so that
IV. APPLICATION TO PLANAR SYSTEMS
A. Wave equation and normalisation formula in 1D
IV. APPLICATION TO PLANAR SYSTEMS
In this sub-section I consider how Maxwell's wave equation transforms to 1D. I also consider how the normalisation formula transforms to 1D.
IV. APPLICATION TO PLANAR SYSTEMS
Maxwell's wave equations for a planar dielectric structure with permeability µ = 1 surrounded by vacuum is reduced for 1D to the following equation:
IV. APPLICATION TO PLANAR SYSTEMS
We take the transverse eigen-modes with index n to have zero in-plane wave number. The eigen-modes can be factorised as
IV. APPLICATION TO PLANAR SYSTEMS
with time independent part satisfying the wave equation:
IV. APPLICATION TO PLANAR SYSTEMS
The electric field and its first derivative are continuous everywhere. Eigenmodes of Maxwell's wave equation for open systems have outgoing boundary conditions. In 1D non-dispersive systems the RSs E n (z) with frequency k n are orthogonal and normalized correctly in 1D according to [3] a −a
IV. APPLICATION TO PLANAR SYSTEMS
where z = ±a are the positions of the boundaries of the unperturbed system.
B. Resonant states of the unperturbed slab
In this sub-section I give the RSs used to calculate the RSE Born approximation in Sec. V.
B. Resonant states of the unperturbed slab
Solving the wave equation Eq. (25) for dielectric constant ε(z) given by Eq. (22), the electric field of RS n, normalized according to Eq. (26), takes the form [3] 
B. Resonant states of the unperturbed slab
where
B. Resonant states of the unperturbed slab
with
B. Resonant states of the unperturbed slab
and
B. Resonant states of the unperturbed slab
the imaginary part of the wave vectors k n are all the same.
C. The form of the RSE Born approximation in the one dimensional case
It is demonstrated in this section that the 1D RSE Born approximation can be used in conjuncture with the RSE perturbation theory (to generate the normalised eigen-modes of planar systems with arbitrary dielectric profile and dispersion) [3, 4, 6, 12] to offer a possible alternative to the scattering matrix method of Ref. [17] . The same method for planar waveguides can be developed in an analogous way except the eigen-modes should be calculated as in Ref. [6, 12] .
C. The form of the RSE Born approximation in the one dimensional case
In 1D the GF G k (z, z ′′ ) is the solution of the equation
C. The form of the RSE Born approximation in the one dimensional case
which from Eq. (4) we can see is given by
C. The form of the RSE Born approximation in the one dimensional case
The free space GF is a solution of
C. The form of the RSE Born approximation in the one dimensional case
and is given by
C. The form of the RSE Born approximation in the one dimensional case
Hence in 1D the RSE Born approximation is greatly simplified to
C. The form of the RSE Born approximation in the one dimensional case
where A n is defined as the Fourier transform,
C. The form of the RSE Born approximation in the one dimensional case
which in the case of a homogeneous slab treated here is calculated to be
C. The form of the RSE Born approximation in the one dimensional case
(37) Interestingly in 1D we do not require the far field approximation to make the simplification of the Green's function required to bring the RSE Born approximation to the form of Eq. (35). Hence in 1D the RSE Born approximation is valid everywhere outside of the slab and not just in the far field. 
V. NUMERICAL VALIDATION
In this section we calculate the 1D GF outside of the homogeneous slab given by Eq. (22) where ǫ s = 2.25. We do this using the RSE Born approximation, analytically using boundary conditions, and also using the spectral GF for comparison. We find that the RSE Born approximation requires less basis states to reach a required accuracy than the spectral GF and unlike the spectral GF is convergent outside the system. I calculate three types of GF in this section, an analytic GF, the GF of Eq. (32) and the GF of Eq. (35). From these it is possible to use the formula derived in Ref. [4, 6] for normal incident and waveguide systems for the transmission T (k, z ′ ),
V. NUMERICAL VALIDATION
The analytic GF is found by solving Maxwell's wave equation in 1D with a source of plane waves while making use of Maxwell's boundary conditions.
V. NUMERICAL VALIDATION
The procedure used to select the basis of RSs for the RSE Born approximation calculation is analogous to that described in Ref. 7 for the RSE perturbation theory. Namely, I choose the basis of RSs such that all RSs with |k n | < k max (N ) using a maximum wave vector k max (N ) chosen to select N RSs.
V. NUMERICAL VALIDATION
From Fig. 1 we can see that unlike the standard Born approximation the RSE Born approximation is valid over From Fig. 2 we can see that unlike the GF calculated with the spectral Eq. (32) the RSE Born approximation is stable over an arbitrarily wide range of z ′ , where z ′ is the coordinate of the point of transmission to, depending only on the basis size N used. The transmission calculated via the spectral GF is diverging with distance of the point of transmission from the slab, this suggests that outside the system the RSE spectral GF is not converging or is divergent. Furthermore we see that the RSE Born approximation requires fewer resonant states than the spectral GF method in order to produce a required absolute error, at all values of z ′ . Although these points were first noted by Ge et al. [2] they were using the unstable normalisation leading to an incorrect GF and so the results upon which they based their conclusions are not reliable.
VI. SUMMARY
In this work we have seen the Born approximation mathematically rigorously extended to include terms which take into account the resonances of the scattering potential using the exact same method as [2] except with correctly normalised modes. Further I have made comparisons in 1D between scattering calculated with the spectral GF and the scattering calculated using the RSE Born approximation. I have demonstrated that once the correct normalisation is used in the RSE Born approximation convergences towards the exact solution is obtained. I have found that the RSE Born approximation for finding the full GF outside of the system is superior to the other spectral GF method considered in terms of convergence and accuracy when the correct normalisation of the RSs is used.
VI. SUMMARY
It is demonstrated in this paper that the 1D RSE Born approximation can be used in conjuncture with the RSE perturbation theory (to generate the normalised eigenmodes of planar systems with arbitrary dielectric profile) [3, 4, 6, 12] to offer a possible alternative to the scattering matrix method of Ref. [17] . In fact, given the superior efficiency of the RSE perturbation theory in comparison with FDTD and FEM for weak perturbations demonstrated in Ref. [7] it is likely that the RSE coupled with the RSE Born approximation will be an incredibly powerful scattering theory for weak scatterers.
VI. SUMMARY
I have now derived an analogous theory for general wave equations [12] . In order to simplify the RSE Born approximation and develop Eq. (6) we require an appropriate spectral form of the GF which is different from the one already proven in the literature. To obtain this correct form I start with the GF valid inside the scatterer only, which I derived in Ref. [5, 12] 
VI. SUMMARY
gives for k → ∞,
VI. SUMMARY
since throughout the derivation in this appendix we are considering the limit where k → ∞ at whichε k (r) = ε(r), i.e. the system is non-dispersive at high frequencies. Convoluting Eq. (A3) with arbitrary finite functions and assuming the series are convergent we see that since k → ∞ we have the sum rule,
VI. SUMMARY
Combining Eq. (A1) and Eq. (A4) yieldŝ
VI. SUMMARY
Combining Eq. (A3) and Eq. (A4) leads to the closure relationε
VI. SUMMARY
which expresses the completeness of the RSs, so that any function can be written as a superposition of RSs. If in the perturbed system some of the series are not convergent or are instead conditionally convergent then we will not arrive at the sum rule and completeness, in which case I expect that the RSE Born approximation will still give convergence to the exact solution but only if a valid spectral Green's function is used, such as Eq. (A1).
Appendix B: RSE for dispersive systems
Due to the problems with non-convergence of Schur factorisation for the generalised eigen-value problem of perturbing nano-spheres dispersively, the RSE in Ref. [11] might tends to fail for non-symmetric perturbation when more than typically 500 basis states are used. This is an estimate based on the un-reported RSE failures for half and quarter sphere perturbations using the generalised eigen-value problem form of the RSE, tests which I carried out for Ref. [7] . Therefore it is necessary to add linear dispersion through a second stage perturbation, a perturbation to the possibly complex conductivity [11] .
Appendix B: RSE for dispersive systems
To make this perturbation consider the problem of a perturbation to the conductivity −i∆σ(r)/k µ
Appendix B: RSE for dispersive systems
ε kµ could have in principle any dispersion for which the eigen-modes can be normalised, and which becomes nondispersive in the limit of high frequency in order to make the sum rule for the GF. In this Appendices Greek index letters denote perturbed modes and British (English) lower case index letters denote unperturbed modes.
Appendix B: RSE for dispersive systems
Since
Appendix B: RSE for dispersive systems
whereĜ kµ (r, r ′ ) is given by Eq. (A5) and by Eq. (A6)
Appendix B: RSE for dispersive systems
where in Eq. (B3) E n and k n correspond to the unperturbed modes of Eq. (5), then following the derivation method of Ref. [8, 9] 2b
Appendix B: RSE for dispersive systems
where
Appendix B: RSE for dispersive systems
which can be solved for the eigen-modes E µ and eigenvalues k µ of the perturbed problem. For examples of fitting dispersion linear in wavelength to the dispersion of real materials for the purposes of RSE perturbation theory please see my Ref. [11] where a linear dispersive RSE is presented in terms of a generalised eigen-value problem.
Appendix B: RSE for dispersive systems
The perturbation toε kµ can also be non-dispersive without resorting to generalised eigen-value problems, as treated in my Ref. [7] . To elaborate further on this point consider the problem of the non-dispersive perturbation ∆ε(r)
Appendix B: RSE for dispersive systems
Againε kµ is dispersive as in Eq. (B1). Eq. (B6) is solved by [7] 
Appendix B: RSE for dispersive systems
where
Appendix B: RSE for dispersive systems
and b nµ √ k n = c nµ . Please note that it is very important to be consistent with the signs of √ k b in the matrix elements of Eq. (B7).
Appendix B: RSE for dispersive systems
Using the linear eigen-value approach outlined here it might be possible to treat an unperturbed Drude-Lorentz gold sphere with a non-dispersive shell, and perturb away the non-dispersive shell leaving in its place biological particles to be sensed as a perturbation. All perturbations must be within the boundaries of the unperturbed system due to convergence of the GF, see Fig. 2 .
Appendix B: RSE for dispersive systems
For a discussion of the eigen-functions of Maxwell's equations in spherical coordinates please see [21] .
Appendix C: Kristensen normalisation
In order for the normalisation of Kristensen et al to be correct it must be consistent with my Eq. (6), specifically the surface term S RSE in Eq. (6) must be mathematically equivalent with Kristensen's surface term S KS . Hence it should be that S RSE = S KS , where from [3] we have,
Appendix C: Kristensen normalisation
and from Eq. (7) we have
Appendix C: Kristensen normalisation
However considering the RSE Born approximation in 3D, specifically to ensure outgoing BCs Eq. (17) in particular driven by (convoluted with) a current vanishing proportional to (k − k n ) as k → k n so E(r) → E n (r), we know that
Appendix C: Kristensen normalisation
where r = (r, θ, φ) in spherical polar coordinates and f (θ, φ) ∝ A n (rk n ), then substituting Eq. (C3) into Eq. (C1) and Eq. (C2) and equating S RSE and S KS gives,
Appendix C: Kristensen normalisation
a logically valid statement, therefore, S RSE = S KS when r → ∞ and so the normalisation of Kristensen et al is not wrong as it is stated. In the RSE perturbation theory letting r → ∞ in the normalisation of perturbed modes introduces huge errors because of the blow up of the RS mode fields far from the system causing blow up of error. By Eq. (C4), as r grows one is essentially subtracting an exponentially growing surface term from an exponentially growing volume term to get the constant 1 + δ kn,0 for normalisation, this leads to large numerical errors for low-Q (leaky) modes [13] . An inherent source of instability is remaining dependence of f (θ, φ) on r due to the use of finite r.
Appendix C: Kristensen normalisation
In 1D Kristensen et al normalisation is actually correct for any finite r that includes the system inhomogeneity [3] .
Appendix C: Kristensen normalisation
The remaining problems with the Kristensen et al normalisation is that it is missing k = 0 modes, therefore it is incomplete, and hence incorrect. Also it does not have the conditions onε k which should be the same as for my normalisation. That the RSs can be written in the form of Eq. (C3) aids the solution of the inverse scattering problem [12] .
Appendix C: Kristensen normalisation
As an aside, since
Appendix C: Kristensen normalisation
it is theoretically possible to make calculations of the potential from the emission (decay) via fast inverse Fourier transform methods upon the set of A n (rk n ) especially if the potentials of interest are rotating about a fixed axis so we know their orientation to some extent such as occurs for decaying magnetic nuclei as part of a nonmagnetic crystalline compound placed inside a NMR (nuclear-magnetic-resonance) machine. Because k n are discrete values these inverse Fourier methods might have to be used self-consistently in conjuncture with the RSE perturbation theory and the values of k n . This is a highly speculative aside and might be a possible topic for future research.
Appendix C: Kristensen normalisation
As another aside, close to a sharp resonance k ≈ k n scattering from the potential is dominated by a single resonance and so the scattered E-field E scattered is approximately
Appendix C: Kristensen normalisation
again A n (rk) can be partially inverse Fourier transformed with respect to angle to find information about the internal structure of the potential. C is some constant. This argument assumed elastic scattering, which is a valid assumption even for such things as neutronnucleus scattering provided that the neutron energies are high enough, at low energies inelastic scattering causes deviations from the RSE Born approximation model, these deviations in scattering caused by inelasticity give the fission or absorption cross-sections. An RSE for Schrödinger's equation is given in [12] . For 2D systems, by following similar arguments as here we arrive at (in the notation of [12] )
Appendix C: Kristensen normalisation
and the arguments with regards to normalisation in this Appendix C still hold except that now

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