Tests of Quantum Gravity induced non-localityvia opto-mechanical quantum oscillators

Tests of Quantum Gravity induced non-locality
via opto-mechanical quantum oscillators

Alessio Belenchia abelen@sissa.it    Dionigi M. T. Benincasa dionigi.benincasa@sissa.it    Stefano Liberati liberati@sissa.it SISSA, Via Bonomea 265, I-34136 Trieste, Italy and INFN, Sez. di Trieste.    Francesco Marin marin@fi.infn.it Dipartimento di Fisica e Astronomia, University of Florence, Via Sansone 1, I-50019 Sesto Fiorentino, Firenze, Italy and INFN, Sez. di Firenze. European Laboratory for Non-Linear Spectroscopy (LENS), Via Carrara 1, I-50019 Sesto Fiorentino, Firenze, Italy.    Francesco Marino marino@fi.infn.it CNR-Istituto Nazionale di Ottica, Largo E. Fermi 6, I-50125 Firenze, Italy and INFN, Sez. di Firenze.    Antonello Ortolan antonello.ortolan@lnl.infn.it INFN, Laboratori Nazionali di Legnaro, Viale dell’Università, 2, 35020 Legnaro, Padova, Italy.
Abstract

Several quantum gravity scenarios lead to physics below the Planck scale characterised by nonlocal, Lorentz invariant equations of motion. We show that such non-local effective field theories lead to a modified Schrödinger evolution in the nonrelativistic limit. In particular, the nonlocal evolution of opto-mechanical quantum oscillators is characterised by a spontaneous periodic squeezing that cannot be generated by environmental effects. We discuss constraints on the nonlocality obtained by past experiments, and show how future experiments (already under construction) will either see such effects or otherwise cast severe bounds on the non-locality scale (well beyond the current limits set by the Large Hadron Collider). This paves the way for table top, high precision experiments on massive quantum objects as a promising new avenue for testing some quantum gravity phenomenology.

pacs:
04.60.Bc, 07.10.Cm, 42.50.Wk

Introduction.—A vast uncharted territory lies between the scale presently tested in high energy accelerators, eV, and the Planck scale, eV, where quantum gravitational physics is expected to become relevant. Quantum gravity phenomenology is a broad field of research which attempts to bridge this gap by connecting models of quantum gravity with observation/experiments. In the absence of a definitive theory of quantum gravity, much of the present literature has resorted to testing general ideas ensuing from various models, ranging from large extra dimensions Hossenfelder:2003jz (), to generalisations of the uncertainty principle at the Planck scale Garay:1994en (); Hossenfelder:2012jw (), to effective field theories (EFT) implementing a breakdown of Lorentz invariance at the Planck scale Mattingly:2005re (); Liberati:2013xla (), and several others (see also AmelinoCamelia:2008qg () for a more comprehensive review of current proposals).

Within this context, special interest is deserved by those QG scenarios where Lorentz invariance is held as a guiding principle, while spacetime is seen as emerging from more fundamental structures Bombelli:1987aa (). It is generally believed that a successful marriage between fundamental discreteness and local Lorentz invariance (LLI) requires some form of non-locality Benincasa:2010ac (); Gambini:2014kba (). Indeed, disparate approaches to quantum gravity where this marriage occurs explicitly lead to nonlocal modifications of standard local dynamics. Explicit realisations arising from quantum gravity models aside, the appearance of nonlocal dynamics can be expected on very general grounds: LLI together with the the requirement that the dynamics not suffer from classical instabilities, effectively singles out two types of dynamics, standard local dynamics (1st or 2nd order in space and time) and nonlocal dynamics (-order in space and time) — the infinite number of time derivatives being needed in order to avoid Ostrogardsky’s theorem Ostro ().

In particular, let us consider the example of a free scalar field in flat spacetime. Its standard dynamics are given by the Klein-Gordon (KG) equation, i.e. the dynamics are local, and indeed stable. A modification of this dynamical law, which respects LLI and avoids generic Ostrogardsky instabilities, must necessarily take the form , where is some non-polynomial function, i.e. the dynamics become nonlocal, with stability depending on the specific choice of . It follows therefore that if specific models of QG lead to modifications of standard local dynamics while simultaneously claiming to preserve LLI, then they must do so through nonlocal dynamics of the kind just described. Indeed, this expectation is realised in various QG models which hold LLI as a guiding principle Biswas:2014yia (); Koshelev:2011gx (); Sorkin:2007qi ().

The definition of must contain a characteristic, covariantly defined scale, which allows for a suitable power law expansion characterising the deviation from the standard local field equations. It is important to note that this scale, which we refer to as the non-locality length scale, , need not be related to the quantum/discreteness scale normally associated to QG, i.e. the Planck scale. In fact, in various approaches to QG leading to this kind of nonlocal dynamics this will usually be some mesoscopic length scale lying somewhere between the TeV scale and the Planck scale (see e.g. Sorkin:2007qi ()); a fact which is of particular relevance within the context of casting phenomenological constraints.

In what follows we shall describe a novel, promising way to test non-local dynamics of this type. Restricting ones attention to nonlocal effective field theories which are both classically and quantum mechanically stable and, crucially, that can be derived from an underlying quantum gravity theory, effectively singles out nonlocal dynamics defined by an analytic . This does not imply that non-analytic s are not interesting (in fact this case naturally arises in the context of causal set theory Aslanbeigi:2014zva (); Belenchia:2014fda ()), but rather that further investigations in the stability and unitarity of these theories are needed before much effort is invested in extending an analysis similar to the one described below to such cases. A significant consequnce of considering analytic s is that it will allow us to solve the dynamics perturbatively.

We will perform a perturbative study of the effects of modified equations of motion on the evolution of opto-mechanical quantum oscillators based on the following methodological steps. In order to compare our analysis to actual experiments on the aforementioned systems, we must first derive the non-relativistic limit of an effective nonlocal massive scalar field theory with dynamics given by an analytic , showing that the evolution of a quantum system is governed by a modified (nonlocal) Schrödinger equation. This approach allows us to overcome long standing issues about how to relate the evolution of macroscopic objects to the effects of nonlocality arising from a potential discreteness of spacetime. We proceed by performing a perturbative expansion around the local regime adapted to the specific experimental setting we are interested in. We then solve for the evolution of the wave function and compute the behaviour of the relevant physical observables. We show that a characteristic signature due to a periodic squeezing is introduced by the first nonlocal correction. Using this feature we discuss the constraints already available and provide forecasts for those deducible from future experiments. In particular, we establish that sensitivity close to the Planck scale can be achieved, thus severely constraining, or even ruling out, models of QG in which the nonlocality scale is larger than the Planck scale.

Framework.— For the non-relativistic limit of an equation of the form to be physically meaningful and have the usual probabilistic interpretation of the wave function, we require that: a) iff (this property ensures that there exist no classical runaway solutions and, when is entire, no ghosts). b) unitarity of the full nonlocal quantum field theory (QFT) and c) the non-local QFT must possess a global symmetry with a conserved charge which is positive semi-definite in the non-relativistic limit (this condition ensures that a probabilistic interpretation can be given).

For concreteness let us consider now the non-local Lagrangian for a free complex, massive, scalar field

(1)

where , and we assume that is an analytic function so that it can be formally expanded as a power series . Implicit in the definition of is , which in the local limit sends ; in particular .

Upon making the ansatz and taking the limit we find

(2)

where NR stands for non-relativistic, and

(3)

is the usual Schrödinger operator.

Depending on the precise form of the function , the conserved charge associated to the symmetry may or may not be positive semidefinite. As stated in (c), in what follows we will assume that such a condition is satisfied. In any case, one can show NLS () that the conserved current is given by a perturbative expansion in whose zeroth order term is the usual one.

Perturbative expansion.— We shall now consider the case of a harmonic oscillator in 1-dimension whose evolution is assumed to be described by the above non-local Schrödinger equation with a harmonic potential. This study is motivated both by its simplicity and ubiquity in physics, and in view of its application to the actual experiments involving systems that are effectively 1-dimensional.

Hence, we wish to solve the nonlocal equation

(4)

where is a harmonic potential , is the mass of the system and its natural angular frequency and, consistently with the local limit requirement, we write

(5)

where the are dimensionless coefficients.

The introduction of the potential allows one to construct a dimensionless parameter which can be used to define the perturbative expansion. Note that represents the ratio between and the width of the oscillator’s ground-state wavefunction and, through , the mass parameter enters the nonlocal dynamics of the harmonic oscillator breaking the usual scaling. This dependence on suggests that massive quantum systems could be the ideal setting for detecting such non-locality.

In order to keep the notation as clear as possible we will use dimensionless variables111These are defined as . In the main text we have systematically omitted the hats for notational convenience. for which we have

(6)

Given the complexity of such an integro-differential equation, together with the fact that we are only interested in small deviations from the standard local behaviour, we shall assume that the non-local Schrödinger equation admits solutions of the form

(7)

where is a solution to the standard Schrödinger equation with harmonic potential, and higher order terms are suppressed by powers . We are therefore assuming that the nonlocal equation admits as an approximate solution in the sense that (see NLS () for further details). This assumption is based on the intuition that a physically reasonable nonlocal generalisation of the Schrödinger equation should admit solutions which are perturbations of solutions of the local Schrödinger equation. The failure of this property would otherwise put the theory in serious tension with well-tested physics.

We will be interested in perturbations around coherent states, since these are easiest to realise within the experimental settings we have in mind, and furthermore include the harmonic oscillator’s ground state as a specific case. Substituting this back into (6) one finds that the differential equation at order is the standard Schrödinger equation for with a source term depending on the solution to the perturbative problem at order .

At zeroth-order in we have the standard Schrödinger equation with a harmonic oscillator potential for which we choose a solution corresponding to a coherent state, . To solve the equation to first order we make the following ansatz

(8)

Substituting this into equation (6) and keeping only terms of order one finds a system of ODEs for the time dependent coefficients that can be easily solved.

Results.— We present results for perturbations around a generic coherent state obtained by solving the non-local Schrödinger equation perturbatively up to order (the corresponding results for the ground state can be found by setting the coherent amplitude ). Since is not conserved by the first perturbative term, in order to have a well-defined probability distribution we normalise the wavefunction using the norm of , i.e. in accordance with the Born rule we shall define the probability density as

(9)

such that . While for the ground state this normalization factor is one at order , in the case of a generic coherent state an order time dependent correction will be present. The above normalisation factor ensures that even in this case we a have a meaningful probability distribution.

The mean of position and momentum are given by

(10a)
(10b)

At order the variance in position and momentum are given by

(11)
(12)

Note that , which is consistent with the state being a state of minimum uncertainty to first order, although the variances themselves possess a time dependence which leads to a spontaneous time-dependent, cyclic squeezing in both position and momentum, see Fig. 1.

Figure 1: Time dependence of the variances of a coherent state for and . The continuous (blue) and dashed (red) lines represent the position and momentum variances respectively. The black dot-dashed line is the standard value, 1/2, of both variances in the local theory. Below the plot we sketch in phase diagrams the proposed experimental procedure for measuring the variance of , involving (I) cooling the oscillator down to , (II) a pulsed excitation in a well-defined coherent state, (III) free evolution for a time , (IV) the measurement of in a time interval shorter than the oscillation period. Steps (II) and (III) should last much less than the thermal decoherence time. The cycle is iterated several times, the variance of the measurements of is calculated, then is changed and the whole measurement procedure repeated.

Present constraints and forecasts.— We now consider the constraints imposed by both existing opto-mechanical experiments and experiments that will be performed in the near future. Let us begin by noting that bounds on the non-locality scale have already been obtained by comparing nonlocal relativistic EFTs to the 8 TeV LHC data Biswas:2014yia (), in which the authors find m.

Returning to the non-relativistic setting, experiments have recently achieved the goal of cooling a mechanical oscillator down to thermal occupation numbers below unity, i.e. to conditions close to the ground state. In such systems, a wave function can be associated to an effective coordinate describing an elastic vibration mode, or, to reasonable approximation, the center-of-mass of an oscillating portion of a body. The coordinate is measured by a mode of an electromagnetic field (the meter), whose eigenfrequency depends on such coordinate. The interaction can be generally described by a Hamiltonian of the kind , where is the coupling strength that depends on the system’s geometry and is the electromagnetic field’s annihilation operator Aspelmeyer2014 ().

The expressions that we derived contain coefficients, , that depend on the specific model. For the sake of clarity, in the following we set . We start our analysis by comparing the measured variance of with our corresponding prediction for the ground state. Taking the time average of (11), with , we infer that it should differ from its standard value by . For a meaningful comparison, the experimental system needs to be well within the perturbative regime, i.e. . This implies that the experiment should achieve an oscillator energy close to its standard ground value (namely with an average occupation number ). In these conditions, Eq. (11) allows one to derive an upper limit to of the form .

The experiments with macroscopic oscillators that enter the quantum regime more deeply (Ref. OConnell2010 () achieved and Ref. Meenehan2015 () achieved ), do not provide a measurement of the variance of . Other experiments teufel2011sideband (); wollman2015quantum (); Pirkkalainen2015 (); Lecocq2015 (), which use the drum mode of aluminum membranes, measure instead of the oscillator coupled to microwave radiation that is used to cool and monitor its motion. In the best case scenario, with  Lecocq2015 (), Eq. (11) yields the upper limit . Using  fm (the mass is  pg teufel2011sideband () and the frequency  MHz), we derive  m. This is reasonably close to the constraint obtained at LHC and has the extra virtue of being independent of it.

A further comparison between our theory and experiments can be based on the evolution of coherent states. As shown in Eqs. (10a)-(10b), our model predicts some third-harmonic distortion proportional to and : the effect of non-locality is thus amplified, with respect to the ground state, by the coherent amplitude . Unfortunately, to our knowledge no experiment could so far realise a quantum coherent state, i.e. a coherent state produced from the ground state, where thermal fluctuations are negligible. Treating such cases rigorously would require a generalisation of Eq. (10a)-(10b) to thermal states, something far from being straightforward.

However, the situation is not as hopeless as it might seem. A recent set of experiments developed highly isolated quantum oscillators, i.e. with a high mechanical quality factor, to constrain potential Planck scale deviations from the standard uncertainty relations Bawaj:2014cda (). These systems also suffer from the issue of only being able to generate thermal coherent states, but are presently undergoing improvements which should allow them to enter a truly quantum regime.

Interestingly, we can already provide first estimates of the strength of the constraints achievable via these experiments. In Ref. Bawaj:2014cda (), the oscillator is excited in order to create a coherent state with large amplitude , then the time evolving position is monitored through weak coupling to a meter field. The third-harmonic component of is accurately evaluated as a function of . Such third-harmonic should be null in a perfectly harmonic oscillator, with standard dynamics. On the contrary, its presence is predicted by Eqs. (10a), namely with a ratio between third- and first-harmonic amplitudes (third-harmonic distortion) equal to . A third harmonic can also be interpreted as a consequence of the deformed commutator analysed in Ref. Bawaj:2014cda (), with a third-harmonic distortion equal to where is a deformation parameter.

A non-null third-harmonic distortion is indeed found in Ref. Bawaj:2014cda (), and it is explained as the effect of structural non-linearities. Assuming no accidental cancellation between non-linearities and deformed dynamics, and attributing, in the worst case, the overall effect to the deformed dynamics, Ref. Bawaj:2014cda () derives a series of upper limits for for different oscillator parameters (frequency and mass). Comparing the above expressions for the third-harmonic distortion, we can directly translate the upper limits on to upper limits on () and (). Such limits range from m (for an oscillator with  kg and  Hz), to m ( kg and  Hz).

Such figures suggest that similar experiments, once performed on pre-cooled, quantum oscillators — all improvements within technical reach and currently under realisation — could explore the interesting region between the electroweak and Planck scales and cast constraints stronger than those achieved at LHC by several orders of magnitudes. Let us remark that while our best forecast falls short by roughly six orders of magnitude from m, figures of this order could already be effective for constraining scenarios where the non-locality scale is larger than the Planck one.

The experiments just described are useful to set constraints on non-local effects but, should they be observed, can hardly be used to claim the discovery of such phenomena, since a third-harmonic distortion can be attributed to several effects. On the other hand, the spontaneous, oscillating squeezing is a much more meaningful phenomenon that cannot be generated by environmental effects. Of crucial importance for a potential experimental test is that the oscillation has a precise phase relation with the evolution of the average position in a coherent state, a property that can be exploited in synchronous detections.

A realistic experiment could be based on repeated measurement cycles on a mechanical oscillator, including: a) the cooling down to , b) the pulsed excitation in a well-defined coherent state and c) after a delay , the measurement of (see the sketch in Fig. 1). Note that the use of pulsed techniques Vanner2013 (), and the estimate of time-evolving indicators on iterated measurements Pontin2015 (), are indeed at the forefront of experimental research in opto-mechanics. In this sense, we argue that the class of experiments under preparation are already in the right regime to severely constrain (or in the best scenario confirm) non-local physics at sub-Planckian scales.

Conclusions. — In this work we have shown that experiments via opto-mechanical quantum harmonic oscillators can cast very severe constraints on the scale of non-locality associated to several QG scenarios which respect local Lorentz invariance. This was achieved by considering the non-relativistic limit of a non-local EFT characterised by an analytic function of the Klein-Gordon operator. The so derived non-local Schrödinger equation was solved perturbatively in the experimentally relevant case of a harmonic oscillator. The perturbed solutions showed a characteristic periodic squeezing which cannot be introduced by environmental effects or by dissipative behaviour due to the finiteness of the quality factor. This provides a clear signature of what one should seek for in this class of experiments, and opens up a new channel for quantum gravity phenomenology. Improvements of the oscillators reported in Bawaj:2014cda () are under development with the precise aim to test the features presented here. These new experiments will soon reach sensitivities close to the Planck scale, and will therefore offer a concrete possibility of observing quantum gravity induced effects, or at least rule out a whole class of candidate theories.

Acknowledgements.
Acknowledgments. — A.B., D.M.T.B and S.L. wish to acknowledge the John Templeton Foundation for the supporting grant #51876. AB also acknowledges the support of STSM Grant from the COST Action MP1006 and would like to thank F. Dowker and Imperial College for interesting discussions and hospitality during early stages of this work. The authors also thank S. Hossenfelder for useful comments on the manuscript.

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