# Probing Mixing of Photons and Axion-Like Particles by Geometric Phase

Authors: A. Capolupo; G. Lambiase; G. Vitiello
Journal: Advances in High Energy Physics
 (2015)

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## Abstract

We find that a geometric phase characterizes the phenomenon of mixing of photons with axion-like particles (ALPs). The laboratory observation of such a phase may provide a novel tool able to detect such a mixing phenomenon. We show that the geometric phase is dependent on the axion-like particle mass and coupling constant. We discuss an interferometric experiment able to detect the geometric phase associated with the ALPs-photon mixing.


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## Body

## 1. Introduction

In the physics beyond the Standard Model much attention is devoted to the study of ultralight and weakly coupled particles. In particular the axion and axion-like particles (ALPs) and their properties have been thoroughly analyzed. The study of ALPs starts with the assumption of the existence of the axion in order to resolve the strongCP problem in quantum chromodynamics [1, 2]. Such a particle is supposed to be a pseudo-Nambu-Goldstone boson with no electric charge and mass expected to range between 10-6 and 10-2 eV, with very small cross section for strong and weak interactions. An interesting property of the axion and of the ALPs is that they can couple to an electromagnetic field, so that they should mix with photons and oscillate in the presence of strong magnetic fields [3, 4]. Axions and ALPs are proposed to be natural candidates for cold dark matter. Their existence could be revealed in the anomalous cooling of white dwarfs and the anomalous transparency of the Universe for very high energy gamma rays.Different kinds of terrestrial experiments have attempted to detect axions. The proof of their existence is of course a target of primary experimental importance. A small anomalous rotation of the direction of light polarization, propagating through magnetic fields, has been investigated in PVLAS [5]. In CAST, axions of astrophysical origin are searched by using the Primakoff effect [6–8] and, in ADMX, a strong magnetic field permeating a cold microwave cavity [9, 10] has been utilized to reveal the axion presence. The conversion of photons into axions has been also analyzed in a beam of light passing through an intense magnetic field [11–15], although without positive results [11–15]. In cosmology, a recent analysis of axion dark matter scenario has been carried out in [16–18]. It has been shown that the axion and ALP contribution to the dark matter can be obtained provided that the axion mass is ma=(82.2±1.1) μeV or ma=(76.6±2.6) μeV (which correspond to the breaking of the Peccei-Quinn symmetry at a scale fa=(7.54±0.10)×1010GeV or fa=(8.08±0.27)×1010GeV, resp.).In recent years, on the other hand, a great attention has been devoted to the study of topologically nontrivial phases, the so-called geometric phases [19–27]. These are not reducible to or derivable from dynamical phases (neither the vice versa is possible due to their substantial, nonslight, or negligible difference; these ones cannot be written in terms of the other ones) and have been experimentally observed in the evolution of many physical systems, from photons in optical fibers [28] and nuclear magnetic resonance [29] to superconducting circuits [30, 31] and electronic harmonic oscillators [32]. Their possible applications in different fields of physics [33–37] have also been studied extensively. Our experience in computing the geometric phase and its consequences in elementary particle physics, in particular in particle mixing and oscillations [33, 38, 39], has inspired us to consider the emergence of topological phases in axion physics. Preliminary results have been presented as an extended abstract in the conference report of [40].In this paper we show that the mixing of photon with ALP gives rise indeed to the appearance of a geometric phase. Specifically, we demonstrate that the geometric phase represents an observable characterization of the time evolution of photons and ALPs only if their mixing is present. On the contrary, no geometric phases arise in the absence of mixing and/or vanishing external magnetic field. In such cases, the total phase is the dynamical one. Therefore, the conclusion is that the geometric phase could be used as a tool to highlight the generation of axions and ALPs by photons propagating through a strong magnetic field. One, indeed, could measure the difference between the geometric phases associated with two rays of light, propagating in two branches of an interferometer, one through a strong magnetic fieldB and the other one passing through a region, where B=0. In particular, we propose considering a laser beam divided by a beam splitter into two rays of equal intensity, one passing in a region permeated by a strong magnetic field and the other acting as a reference beam passing in a region with no magnetic field. The two photon (laser) beams are then recombined together and might interfere. Indeed, in the presence of photon conversion in ALPs, the beam passing through the region with B≠0 should have a reduced amplitude and a phase shift with respect to the reference beam [41], with the result that there is a reduction in the total intensity of the recombined beam with respect to the original one and an interference pattern due to the difference in the photon phase will appear on the screen.Here we show that the evolution of photon states, in the presence of magnetic field, contains a phase of geometric origin in addition to the usual dynamical phase derived from Schrödinger’s equation. This phase results from the geometrical properties of the parameter space of the Hamiltonian of the system. It is gauge invariant and reparametrization invariant. In the particular case of the mixing of photons with ALPs, the geometric phase depends on the mixing angleθ and therefore on the coupling constant and ALP mass (see below the expression of the mixing angle).The beam of photons which propagates with no interaction with the magnetic field has geometric phase equal to zero. The difference between the geometric phases of the beams exiting from the two branches is then the manifestation of the occurrence of the ALP-photon mixing phenomenon in the branch, whereB≠0.The proposal of such an experiment is new, not drawn from the previous literature. For example, the experiment presented in [42] is based on a different analysis than the one proposed here. In [42] it was proposed to use the interferometer solely to reveal the reduction of the power of the laser beam in the output with respect to the input power, without any consideration concerning the geometrical phases. In the seminal paper [41] the phase in the photon-ALP mixing in the presence of electromagnetic field has been discussed without reference to the geometric phase, which on the contrary is the main focus of the present paper. Our formalism is fully consistent with the analysis of [41], but it also includes the study of the geometric phase arising as a consequence of the photon-ALP mixing. In the Appendix we outline the main contact points of our formalism with [41].We observe that the analysis of the geometric phase applies both to scalar and pseudoscalar ALPs and it can be used to discriminate between the two cases. We consider the pseudoscalar case.The paper is structured as follows. In Section2 we recall the basic formalism describing the axion-photon mixing. In Section 3 we present the geometric phase characterizing such a phenomenon and study its possible application to the detection of axion and of axion-like particles. Section 4 is devoted to conclusions.


## 2. Axion-Photon Mixing

The lagrangian density of the ALP-photon system is given byL=Lγ+La+LQED+Laγγ, where Lγ=-1/4FμνFμν and La=1/2(∂μa∂μa-ma2a2) are the lagrangian densities of free photon and axion; LQED=α2/90me4[(FμνFμν)2+7/4(FμνF~μν)2] is the Heisenberg-Euler term due to loop correction in QED [43–45], which we neglect in the approximation we consider. Laγγ is given by (1)Laγγ=gaγγ4aFμνF~μν, and it represents the interaction of two photons with the axion pseudoscalar field a in the presence of a magnetic field [46]. Equation (1) can be written as Laγγ=-gaγγaE·B. Here F~μν=1/2ϵFμνρσρσ is the dual electromagnetic tensor; gaγγ≡g≡gγα/πfa is the axion-photon coupling with dimension of inverse energy, with gγ being of the order of the unity, α=1/137, and fa being the decay constant of ALPs. By means of such an interaction, axion and photon can mix with each other in a background magnetic field.We consider a monochromatic laser beam splitted into two beams, one propagating through a region permeated by a magnetic field and the other traversing a region withB=0. The two beams exiting from the two branches are then recombined together. We assume that the beam propagating in the presence of the magnetic field has the direction along the z-axes. Besides the LQED term, we also neglect the birefringence of fluids in a transverse magnetic field (Cotton-Mouton effect). With these simplifications, choosing the y-axis along the projection of B perpendicular to the z-axes, the photon polarization state γx=γ⊥ decouples and the propagation equations can be written as (2)ω-i∂z+Mγ∥a=0, with B=BT; purely transverse field and mixing matrix M are given by (3)M=-12ωωP2-gωBT-gωBTma2. Here ωP is the plasma frequency and ma is the axion mass. The matrix M can be diagonalized by a rotation to primed fields: (4)γ∥′za′z=cos⁡θsin⁡θ-sin⁡θcos⁡θγ∥zaz. The mixing angle is θ=1/2arctan⁡2gωBT/ma2-ωP2; moreover γ∥′(z)=γ∥′(0)e-iωγz, a′(z)=a′(0)e-iωaz, where(5)ωγ=ω+Δ-,ωa=ω+Δ+,Δ±=-ωP2+ma24ω±14ωωP2-ma22+2gωBT2. In this way, the photons can be converted into ALPs in the branch of the interferometer in which B≠0. The conversion of photons in ALPs manifests itself in a reduced amplitude of that beam and in the phase shift with respect to the reference beam.For the mixing components one has(6)γ∥zaz=Mzγ∥zaz, where (7)Mz=cos⁡θ-sin⁡θsin⁡θcos⁡θe-iωγz00e-iωazcos⁡θsin⁡θ-sin⁡θcos⁡θ. Using (7), γ∥(z) is obtained as(8)γ∥z=e-iωγzcos2⁡θ+e-iωazsin2⁡θγ∥0+cos⁡θsin⁡θe-iωγz-e-iωaza0.Similarly the expression for a(z) is obtained by using (6) and (7). By assuming that the contribution coming from the amplitude a(0) of the axion field is negligible with respect to the γ-term in the right-hand side of (8), we have (9)γ∥z=M11zγ∥0=e-iωγzcos2⁡θ+e-iωazsin2⁡θγ∥0.We observe that the correspondence between the notation of [41] and our notation is Δ∥=-ωP/2ω, Δa=-ma/2ω, and Δ∥′=Δ+, Δa′=Δ-. By following [41], we may neglect the phase e-i(ω+Δ∥)z which is common to γ∥(z), γ⊥(z), and a∥(z); the matrix M(z) becomes(10)Mz=cos⁡θ-sin⁡θsin⁡θcos⁡θe-iΔ∥′-Δ∥z00e-iΔa′-Δ∥zcos⁡θsin⁡θ-sin⁡θcos⁡θand the states (9) are then(11)γ∥z=e-iΔ∥′-Δ∥zcos2⁡θ+e-iΔa′-Δ∥zsin2⁡θγ∥0.In the following section we focus our attention on the geometric phase generated in the laser beam which has been propagating through the branch with the magnetic field. The photon beam carrying such a phase, exiting from such a branch, will then interfere with the photon reference beam.In closing this section, we observe that it has been shown [7] that the transition rate can be enhanced by filling the conversion region with a buffer gas. This induces an effective photon mass mγ. The plasma frequency ωP=(4παNe/me)1/2, where Ne denotes the electron density, plays the role of mγ [7].


## 3. Geometric Phase and Axion-Photon Mixing

In order to show that a geometric phase arises in the evolution of the ALP-photon system, that is, in the laser beam passing through the magnetic field, we use the definition of Mukunda-Simon (geometric) phase [25]. Let us therefore briefly introduce such a definition.Such a phase, derived within a kinematical approach, is associated with any open curve of unit vectors in Hilbert space. For a quantum system whose state vectorψs belongs to a curve C, with s being real parameter such that s∈[s1,s2], the Mukunda-Simon phase is defined as [25] (12)ΦC=arg⁡ψs1∣ψs2-I∫s1s2ψs∣ψ˙sds, where the dot denotes the derivative with respect to the real parameter s. The right-hand side of (12) is the first term in (2.11) of [25]. In (12), arg〈ψ(s1)∣ψ(s2)〉 represents the total phase, while I∫s1s2‍〈ψ(s)∣ψ˙(s)〉ds is the dynamical one. The difference between the two, if not zero, is by definition the geometric phase.To our knowledge the geometric phase has not been considered in [41] and in other existing literatures relative to axion and ALPs. The definition in (12) can be applied to the photons interacting with the magnetic field. In this case, the geometric phase is given by (13)Φγz=arg⁡γ∥0∣γ∥z-I∫0zγ∥z′∣γ˙∥z′dz′, with |γ∥(z)〉 being the state of the photons. For γ∥(z), given by (11), we obtain(14)Φγz=arg⁡e-iΔ∥′-Δ∥zcos2⁡θ+e-iΔa′-Δ∥zsin2⁡θ+Δ∥′-Δ∥cos4⁡θ+Δa′-Δ∥sin4⁡θz-14sin2⁡2θcos⁡Δosczcos⁡2θ, with Δosc≡Δ∥-Δa (as in the notation of [41]). Let us introduce the notation A=1+θ2(cos⁡Δoscz-1) and B=-θ2(Δoscz-sin⁡Δoscz). We then consider (14) at the second order in the mixing angle θ and obtain(15)iΦγz=π2+θ2Δoscz+cos⁡Δoscz,forA=0,B>0,iiΦγz=3π2+θ2Δoscz+cos⁡Δoscz,forA=0,B<0,iiiΦγz=θ22Δoscz-sin⁡Δoscz+cos⁡Δoscz,forA>0,B≥0,ivΦγz=θ22Δoscz-sin⁡Δoscz+cos⁡Δoscz+2π,forA>0,B<0,vΦγz=θ22Δoscz-sin⁡Δoscz+cos⁡Δoscz+π,forA<0,∀B.The nonvanishing value of the geometric phaseΦγ indicates univocally the existence of the ALP-photon mixing phenomenon. Indeed, Φγ(z)=0 when the the magnetic field is zero and the mixing angle θ is equal to zero. This is the case of the reference beam. See the Appendix for a comparison of (14) with the phase definition in [41].The geometric phase is thus calculated for the mixed photon state. It can be detected in the end crossing point of the laser beams (in which the magnetic field is zero), by analyzing the interference between the laser beam passing through the magnetic field and the reference beam. Indeed, the geometric phase accumulated by the photons during their paths through the magnetic field survives when the photons exit the magnetic field and interfere with the reference beam.Notice that the geometric phase can be detected in interferometric experiments when the dynamical phase is much smaller than the geometric one. In general, paths of slightly different lengths can be chosen so that the geometric phase dominates over the dynamical one. In the particular case of the mixing, the phase acquired in the branch withB≠0 will have both a geometrical and a dynamical component. The total phase is (16)ΦTOTB≠0z=Φγz-Δ∥′-Δ∥cos4⁡θ+Δa′-Δ∥sin4⁡θz+14sin2⁡2θcos⁡Δosczcos⁡2θ≃Φγz+θ2Δoscz+cos⁡Δoscz, where the second term on the right-hand side is the dynamical phase in the presence of mixing. On the contrary, the phase of the beam passing in the B=0 branch contains only the dynamical phase: (17)ΦTOTB=0z=Δ∥′-Δ∥z=-Δoscz21-1cos⁡2θ≃θ2Δoscz.By accurately designing the interferometer, the length of the two branches can be linked by the relation(18)lB=0=ΔosclB≠0+cos⁡ΔosclB≠0Δosc.Building the interferometer in this way, once the two laser beams are recombined at the detector, the phase difference will be given by the geometric component. The contributions of the dynamical phases of the two beams, in this case, will indeed compensate each other sinceΔosclB=0=ΔosclB≠0+cos(ΔosclB≠0) and the phase difference ΔΦ will in practice coincide with the geometric phase Φγ induced by the mixing; that is, ΔΦ=Φγ.The interferometer can be built in a way that the beams traverse the branches back and forth many times before recombining at the detector. This can be achieved by suitable use of the mirrors. In this way, the phase will add many times. In principle, one can obtain effective branches of arbitrary length. In the particular case in which the photons interact with the magnetic field in a region of length the order of the axion-photon oscillation lengthlosc=2π/Δ∥-Δa, the geometric phase (14) reduces to the Berry-like phase [19]:(19)Φγz=losc=2πsin2⁡θ.Equation (19) can be then rewritten for the n-cycle case as (20)Φγnlosc=2nπsin2⁡θ≈2ng2B2ω2ma2-ωP22. A Fabry-Perot cavity can be also used in order to enhance the power of the laser light beam.For our estimations, we will utilize (14) and use the following values of the parameters entering the above equations: magnetic field B=10T≃1.95×10-15GeV2, energy ω=10eV, coupling constant g∈[10-16,10-10]GeV−1, axion mass ma∈[10-6,10-2]eV, and plasma frequency ωP=0.9ma.If the experiment runs for the time intervalt=24 hours, we can obtain observable values of the phases ΔΦ as function of the masses and of g. Notice that, as observed in [41], only the photon component of the beam is reflected by mirrors, since any physical mirror is transparent to axions. After N reflections the compound effect is ϕ(L)=Nϕ(l), with L=Nl and l being the distance between the reflecting mirrors [41].By fixing the values of the ALP mass and varying the values ofg, we obtain the following results for the geometric phase:(21)ima~10-2eV,g∈10-11,10-10GeV-1⟶ΦγNl∈10-9,10-7π,iima~10-3eV,g∈10-12,10-10GeV-1⟶ΦγNl∈10-8,10-4π,iiima~10-4eV,g∈10-14,10-10GeV-1⟶ΦγNl∈10-8,1.6π,ivma~10-5eV,g∈10-15,10-10GeV-1⟶ΦγNl∈10-6,0.9π,vma~10-6eV,g∈10-16,10-10GeV-1⟶ΦγNl∈10-4,0.6π.These values ofΦγ(Nl) show that the geometric phase is dependent on the value of the axion mass and on the coupling constant g. Such values are detectable; therefore the geometric phase could represent a new tool to reveal the existence of ALPs and also to provide a region of exclusion for the parameter characterizing the ALP physics.One could wonder that the running timet=24h is too long in order for our system to survive against decoherence phenomenon. However, as in the interferometry experiment proposed by Tam and Yang [42], one may consider running time as long as several days (10 days, 240h, in [42]) provided that one uses laser beams, as it is indeed in our proposed experiment. On the contrary, this would not be the case by considering noncoherent light, which would be trapped in between mirrors in optical cavity systems for a time interval ≪1 sec.The present technologies allow for phase measurements within a precision of ~10−9 [47–49]. Then, the values of the geometric phase here obtained are detectable, provided that sufficient intensity of the signal and signal-to-noise ratio are obtained (see below).Summing up, the presence of a nontrivial geometric phase of the photon demonstrates the presence of axion-photon mixing; it is highly sensible to the axion mass andg and it allows deriving a region of exclusion for the values of the parameters characterizing the axion physics.We also observe that the so-called Schottky (or shot) noise, associated with the particle nature of light, affects the sensibility of the interferometer. In the standard case, the shot noise for photons from laser light represents the relative fluctuations in the photon number per unit time and it can be significant when the number of photons is small [50]. The magnitude of the shot noise increases as the square root of the expected number N of photons. The signal-to-noise ratio is given by r=N/N=N[50]. In the case of the axion-photon mixing, the probability of their conversion is (gBL)2/4, which is obtained for axion mass much smaller than the energy of photons. The signal-to-noise ratio is then given by (gBL)2N/4N. However, in a squeezed state, the number of photons measured per unit time can have fluctuations smaller than the square root of the expected number of photons counted in that period of time [51]. This implies the possibility to increase the sensibility of the interferometer if squeezed light is used in the experiment [52, 53].A nonclassical noise reduction of almost 13 dB below vacuum noise has been observed [54]. Thus, the squeezed light technique has a great application potential. Injected into an interferometer, the quantum noise reduction corresponding to an increase of a factor 10 in laser light power is possible. The use of Fabry-Perot cavity (FPC) in the arms of the interferometer can further increase the sensitivity of the measurements. We stress that a tipical precision in phase measurement, of the order of 10-9, does not in general guarantee the detectability of the phase, which also depends on the intensity of the signal and in turn on the (small values of the) mixing angle, that is, on g. In this connection, in designing the interferometer, we expect that also in our case the strategy outlined in [42] might be adopted in order to boost the sensitivity; namely, one can incorporate in our setup optical delay lines or Fabry-Perot cavities in order to enhance the signal by a factor given by the number of times the laser beam is reflected back and forth in the FPC. By using the estimation made in [42], one might improve the signal-to-noise ratio even by ten dB provided that one uses squeezed laser beams as already mentioned above.


## 4. Conclusions

We have shown that the axion-photon mixing exhibits a characterizing geometric phase. The existence of the geometric phase for photons propagating in a magnetic field signals unequivocally the occurrence of the axion-photon mixing and may provide a novel tool in the detection of such a phenomenon. The relation between axion mass and coupling constant could be tested in a dedicated interferometer experiment.For appropriate values of the photon energiesω and magnetic fields B, the geometric phase could provide a parameter window where searching for ALP contributes to cold dark matter and possible contributions of particle mixing phenomena to the Universe dark energy [55–58].



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