A note on BPS vortex bound states

# A note on BPS vortex bound states

A. Alonso-Izquierdo W. Garcia Fuertes J. Mateos Guilarte Departamento de Matematica Aplicada, Universidad de Salamanca, SPAIN Departamento de Fisica, Universidad de Oviedo, SPAIN Departamento de Fisica Fundamental, Universidad de Salamanca, SPAIN
###### Abstract

In this note we investigate bound states, where scalar and vector bosons are trapped by BPS vortices in the Abelian Higgs model with a critical ratio of the couplings. A class of internal modes of fluctuation around cylindrically symmetric BPS vortices is characterized mathematically, analysing the spectrum of the second-order fluctuation operator when the Higgs and vector boson masses are equal. A few of these bound states with low values of quantized magnetic flux are described fully, and their main properties are discussed.

###### keywords:
Abelian Higgs model, Sel-dual (BPS) vortices, Boson-Vortex bound states

## 1 Introduction

Very soon after the discovery of Abrikosov quantized flux lines in the Ginzburg-Landau theory of Type II superconductors Abrikosov (), the existence and nature of fermionic bound states on these vortex filaments were discussed by de Gennes et al. in Reference deGennes () . Quantized magnetic flux lines were rediscovered by Nielsen and Olesen in the Abelian Higgs model, see Nielsen (), a finding that enhanced the interest of these topological defects by promoting them to the relativistic and quantum world. By adjusting the couplings in the Abelian Higgs model to drive the system to the critical point between Type II and Type I superconductors, Bogomolny showed, see Bogomolny (), that quantized vortex lines still exist but move without interaction with respect to each other. Bosonic vortex bound states were investigated by Goodman and Hindmarsh, see Hindmarsh (), in the context of the Abelian Higgs model for any value of the parameter governing the transition between Type I and Type II superconductivity. In this short note we shall focus on finding BPS vortex bound states and we shall describe these internal boson-vortex modes by a mixture of analytical and numerical methods, at least at the same level of numerical precision as the BPS vortex solutions themselves.

## 2 BPS vortex fluctuations

The Abelian Higgs model describes the minimal coupling between a -gauge field and a charged scalar field in a phase where the gauge symmetry is broken spontaneously . In fact, it is a relativistic version of the Ginzburg-Landau theory of superconductivity. At the transition point between Type I and II superconductivity, where the masses of the Higgs and vector fields are equal, the AHM action reads

 S[ϕ,A]=∫d4x[−14FμνFμν+12(Dμϕ)∗Dμϕ−18(ϕ∗ϕ−1)2]. (1)

Here, non-dimensional coordinates, couplings and fields are used, while is a complex scalar field and is the vector potential. The covariant derivative is defined in the conventional form, , whereas the electromagnetic field tensor is also standard: . We choose the metric tensor in Minkowski space as , , and use the Einstein repeated index convention. In the simultaneous temporal and axial gauges , the Bogomolny arrangement of the energy per unit length for static and -independent field configurations , see Bogomolny (), shows that solutions of the first order PDE system

 D1ϕ±iD2ϕ=0,F12±12(ϕ∗ϕ−1)=0, (2)

with appropriate asymptotic behaviour at infinity in the -plane, are absolute minima of . It was proved in Taubes () that there exist solutions of the PDE’s (2) with finite string tensions that are proportional to the magnetic flux along the -axis of quanta: . These topological objects are denoted BPS vortices because they correspond to the Abrikosov-Nielsen-Olesen vortex filaments arising in Type II superconductors, see Abrikosov ()-Nielsen (), when the scalar and vector penetration lengths in the Ginzburg-Landau free energy are equal and the system lives exactly at the transition point to Type I materials.

Denoting the BPS vortex fields as:

and assembling the vector and scalar vortex fluctuations , in a column vector with transpose

 ξt(→x)=(a1(→x)a2(→x)φ1(→x)φ2(→x))t,

one checks that the linearized dynamics is governed by the action of the second-order vortex fluctuation operator

 H+=⎛⎜ ⎜ ⎜ ⎜ ⎜ ⎜⎝−Δ+|ψ|20−2D1ψ22D1ψ10−Δ+|ψ|2−2D2ψ22D2ψ1−2D1ψ2−2D2ψ2−Δ+12(3|ψ|2−1)+VkVk−2Vk∂k−∂kVk2D1ψ12D2ψ12Vk∂k+∂kVk−Δ+12(3|ψ|2−1)+VkVk⎞⎟ ⎟ ⎟ ⎟ ⎟ ⎟⎠ (3)

on . Resolution of the spectral problem , where is a label in either the discrete or the continuous spectrum of , permits the decomposition of as a linear combination of the eigenfunctions.

In the search for bound state (normalizable) eigenfunctions other than zero modes, i.e. assuming that is the scattering threshold, we shall profit from a hidden SUSY structure of . Linear deformation of the PDE system (9), together with the background gauge

 ∂1[ξ(→x)]1+∂2[ξ(→x)]2−ψ1(→x)[ξ(→x)]4+ψ2(→x)[ξ(→x)]3≡∂kak(→x)−ψ1(→x)φ2(→x)+ψ2(→x)φ1(→x)=0, (4)

is encoded in the following first-order PDE operator

 D=⎛⎜ ⎜ ⎜⎝−∂2∂1ψ1ψ2−∂1−∂2−ψ2ψ1ψ1−ψ2−∂2+V1−∂1−V2ψ2ψ1∂1+V2−∂2+V1⎞⎟ ⎟ ⎟⎠, (5)

acting on the space of BPS vortex fluctuations. This operator allows us to embedd in a SUSY Quantum Mechanical system because and we find the following SUSY algebra generated by the supercharge :

 Q2=(Q†)2=0,H=QQ†+Q†Q=(H+=D†D00H−=DD†), (6)

being the SUSY Hamiltonian, while the SUSY partner to is:

 H−=⎛⎜ ⎜ ⎜ ⎜ ⎜ ⎜⎝−Δ+|ψ|20000−Δ+|ψ|20000−Δ+12(|ψ|2+1)+VkVk−2Vk∂k−∂kVk002Vk∂k+∂kVk−Δ+12(|ψ|2+1)+VkVk⎞⎟ ⎟ ⎟ ⎟ ⎟ ⎟⎠. (7)

Except for the eigenfunctions in the kernel of , which are zero modes of , the two operators are isospectral. This supersymmetric structure led to the proof of the Weinberg index theorem on the plane Weinberg ():

 indD=dimKerD=limM→∞TrL2{M2D†D+M2−M2DD†+M2}=2n,

stating that has zero modes in its spectrum: . Moreover, (6) also guarantees that the -spectrum is non-negative, such that the zero modes of are all the ground states of because .

We shall focus on BPS cylindrically symmetric vortex filaments shaped according to the Nielsen-Olesen ansatz:

 ϕ(→x)=fn(r)einθ;rAθ(r,θ)=nβn(r). (8)

We stress that: (1) Cylindrical coordinates are chosen in the -space and the vector potential components are adapted to them. (2) Besides the temporal and axial gauges, the radial gauge is assumed such that the vector field is purely vorticial. (3) The complex scalar field is expressed in polar form.

The first-order PDE system (2) becomes the following ODE system:

 dfndr(r)=nrfn(r)[1−βn(r)],dβndr(r)=r2n[1−f2n(r)]. (9)

The solutions for the radial profiles and , in the -plane and infinitely repeated along the -axis, determine the cylindrically symmetric BPS vortex solutions. The finiteness of the energy per unit length demands that and as .

Some analytical progress in the investigation of the zero-mode fluctuations on BPS cylindrically symmetric vortices was achieved in Weinberg (). Further comprehension of their structure was obtained in References Ruback () and Burzlaff (). Here, the motivation leading several researchers to describe in detail the vortex zero modes came from the study of vortex scattering at low energies within the approach of geodesic dynamics in their moduli space, see e.g. guilarte (). In this note we shall focus on finding and describing excited fluctuation modes in the discrete -spectrum, i.e., internal modes of fluctuation, where the BPS vortex captures scalar and/or vector mesons, an issue not discussed in the literature on the Abelian Higgs model.

## 3 Spectrum of cylindrically symmetric BPS vortex fluctuations

In the search for positive bound states in the discrete spectrum of the operator , the use of supersymmetry is convenient. If , the SUSY structure (6) implies that . Moreover, the eigenfunctions of are related through the supercharges: . In addition, it should be recalled that the background gauge condition must be satisfied in order to eliminate spurious gauge fluctuations. The strategy is thus to solve the spectral problem for first and apply the operator to the eigenfunctions, finally obtaining the eigenfunctions of . This indirect path is more appropriate because the spectral problem of is more tractable owing to its block-diagonal form. Two classes of eigenmodes of the operator can be distinguished:

Class A -eigenmodes: The two block-diagonal sub-matrix differential operators in prompt a complete decoupling of the vector field from the scalar fluctuations in the -spectral problem. There thus exist eigenfunctions of the form and . The -wave functions of the form do not satisfy the background gauge. Therefore, we shall study only the physically meaningful possibilities among this class of eigenmodes. The non-null component of complies with the PDE , or, in polar coordinates,

 −∂2a1∂r2−1r∂a1∂r−1r2∂2a1∂θ2+[f2n(r)−ω2λ]a1=0. (10)

The separation ansatz 111 , , also leads to (11). We shall pursue the cosine alternative, for the sake of brevity. leads to the 1D Sturm-Liouville problem

 −d2vnk(r)dr2−1rdvnk(r)dr+[f2n(r)−ω2λ+k2r2]vnk(r)=0 (11)

for the radial form factor . Univaluedness of the fluctuations demand that the wave number must be a natural number: . The ODE (11) is no more than a radial Schrdinger differential equation with a potential well , which includes a centrifugal barrier when , bounded below and running to at infinity: . Consequently, a continuous spectrum arises in the range, i.e., for energies above the scattering threshold . Below this threshold, in the range, boson-vortex bound states may exist if the spectral problem (11) admits eigenvalues. The procedure to find both the eigenvalues and the eigenfunctions will be implemented in the next Section for low values of . The need to identify the eigenvalues will leads us to convert the ODE (11), where is a priori unknown, in a system of equations of finite differences by some discretization method of the half-line to a lattice with a finite but large number of points. Diagonalization of the matrix of the linear system in turn provides the eigenvalues and eigenfunctions, which are very good approximations to the eigenfunctions and eigenvalues of provided that the number of points of the discretization is large enough.

Class B -eigenmodes: The block-diagonal sub-matrix in acts only on scalar field fluctuations of the form , leading to the spectral PDE system:

 [−∇2+12(|ψ|2+1)+VkVk]φ1(→x)−2Vk∂kφ2(→x) = ω2λφ1(→x) (12) [−∇2+12(|ψ|2+1)+VkVk]φ2(→x)+2Vk∂kφ1(→x) = ω2λφ2(→x). (13)

For cylindrically symmetric BPS vortices, the ansatz , that converts the PDE system (12) and (13) into the spectral ODE is clear:

 Runk(r)=−d2unk(r)dr2−1rdunkdr+[12(1+f2n(r))+(nβn(r)−(1+k))2r2−ω2λ]unk(r)=0, (14)

where the radial form factor is the unknown. This is a radial Schrdinger differential equation with an effective potential well: . From the functional behavior of , we may conclude that a continuous spectrum arises settled on the threshold value . The same reasoning indicates that there could exist bound states in this class with eigenvalues in the range. However, a theoretical argument can be used to discard this possibility. The linear differential operator associated with the ODE (14) can be factorized as , where refers to the first-order differential operators . This means that the operator has a non-negative spectrum and, consequently, there are no bound states in the discrete spectrum of within this class B of fluctuations.

Translation via use of the supercharges of all the -spectral information described previously reveals the structure of the -spectrum:

Class A -eigenmodes: Assuming knowledge of and from the solution of (11) the eigenfunctions of paired through supersymmetry with these class A -eigenmodes take the form:

 (15)

It is immediate to check that satisfies the background gauge (4), meaning that the fluctuations (15) correspond to admissible eigenfunctions of the second-order BPS vortex fluctuation operator 222The sine alternative leads to degenerate eigenfunctions with obtained by simply replacing by and by in the wave function (15). Knowledge of the radial form factor authomatically gives both the and bound states.. From (11) we may conclude that a continuous spectrum emerges at the threshold value , while the discrete spectrum is confined to the open interval . The presence of bound states in the -spectrum, however, requires the existence of eigenfunctions of (11) satisfying the boundary conditions and . This point will be addressed in the next section.

Class B -eigenmodes: The corresponding SUSY partner -eigenfunctions associated with the class B -eigenfunctions are given by:

The new radial form factor may be defined from the relation in such a way that the ODE (14) turns into the equation

 rh′′nk(r)+[−1−2k+2nβn(r)]h′nk(r)+r[ω2λ−f2n(r)]hnk(r)=0,

for the radial form factor . Regularity at the origin, however, of the positive eigenfluctuations requires that . In this case, there exists a continuous spectrum emerging from the threshold value and no positive eigenvalue bound states arise. Notice, however, that the form of these eigenmodes follow the ansatz given in Ruback () for the zero modes, such that we can regard the zero modes as the only bound class B -eigenmodes 333Other zero modes are easily generated by rotating separately in the scalar and vector field fluctuations, which is a symmetry of the spectral problem. The same argument can be applied to the eigenfunctions ..

Orthogonality between eigenfunctions belonging to different classes is guaranteed by the conservation of the scalar product in the SUSY partnership: , because class A and B eigenfunctions of are clearly orthogonal. Orthogonality between eigenfunctions belonging to the same class with different angular dependence is established by Fourier analysis.

## 4 Positive eigenvalue bound states of the small vortex fluctuation operator

We now attempt to elucidate the existence of excited fluctuations of class A belonging to the discrete spectrum of with positive eigenvalues lower than . The search for and the analysis of these fluctuations reduce to the numerical computation of the radial form factor in the ODE (11). Our strategy to achieve this is to employ a second-order finite-difference scheme that simulates the differential equation (11) by the recurrence relations

 −v(i+1)nk;j−2v(i)nk;j+v(i−1)nk;j(Δx)2−v(i+1)nk;j−v(i−1)nk;j2i(Δx)2+[f2n(iΔx)+k2i2(Δx)2]v(i)nk;j=ω2nk;jv(i)nk;j, (16)

where we have confined the problem to the interval for a large enough . We denote , with , and choose a mesh of points with . The eigenfunctions and the eigenvalues depend on the values of the angular momentum and the vorticity . The index is used to enumerate the discrete eigenfunctions. The contour conditions are:

A good estimation of the discrete eigenvalues is obtained through diagonalization of the matrix in the left member of the linear system (16). We show the eigenvalues of for low values of and obtained in a Mathematica environment in Table 1 by applying this procedure with the choice of . In Figure 1 we illustrate the behavior of the potential wells of the radial Schrödinger equation (11) for and the overlapped dashed lines that determine the discrete eigenvalues of the -spectrum in this case. The radial form factor of the eigenfunctions associated with these eigenvalues are also shown.

In general, we observe that the number of bound states increases with the magnetic flux . In particular, we conclude the existence of 1 bound state for -vortices; 2 bound states for the and vortices; 3 bound states for -vortices, and 4 bound states in the case of -vortices. In Table 1 we include a graphical representation of the discrete -spectrum for several values of the vorticity .

In sum, there exist bound states that are eigenfunctions of . Here, we have described the stationary wave functions where an awkward combination of scalar and vector boson fluctuations are trapped by a cylindrically symmetric BPS vortex. These configurations oscillate in time with frequencies determined by the discrete eigenvalues and are thus internal modes of fluctuation of the BPS -vortex.

## References

• (1)
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• (5) E.B. Bogomolny, “Stability of classical solutions”, Sov. J. Nucl. Phys. 24 (1976) 449
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• (7) A. Jaffe and C. Taubes, “Vortices and monopoles”, Birkhauser, Boston, 1980.
• (8) E.J. Weinberg, “Multivortex solutions of the Ginzburg-Landau equations”, Phys. Rev. D 19 (1979) 3008
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• (11) W. Garcia Fuertes and J. Mateos Guilarte, “Low energy vortex dynamics in Abelian Higgs systems”, Eur. Phys. Jour. C9 (1999) 167
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