Quantum noise in threedimensional BEC interferometry
Abstract
We develop a theory of quantum fluctuations and squeezing in a threedimensional BoseEinstein condensate atom interferometer with nonlinear losses. We use stochastic equations in a truncated Wigner representation to treat quantum noise. Our approach includes the multimode spatial evolution of spinor components and describes the manybody dynamics of a mesoscopic quantum system.
pacs:
03.75.Gg, 03.75.Dg, 67.85.Fg, 67.85.DeAtom interferometry is an important quantum technology at the heart of many proposed future applications of ultracold atomic physics. BoseEinstein condensates (BECs) or atom lasers are macroscopic quantum objects and have potential advantages as interferometric detectors and sensors, provided one can precisely extract atomic phase information. However, unlike photons, atoms can interact strongly, causing dephasing and loss of interference fringes. An intimate understanding of quantum manybody dynamics is the key to calculating interactioninduced dephasing in the measurement process. This is essential for a quantitative theory of atom interferometry.
In this Letter we present a simple, yet quantitatively accurate theoretical approach to simulating the dynamics and evaluating limits of atom interferometry at large atom number, using a truncated Wigner representation Drummond and Hardman (1993); Steel et al. (1998); Sinatra et al. (2002). This method extends the conventional GrossPitaevskii equations describing a Bose condensate to include quantum noise effects, including noise due to linear and nonlinear losses. The theory allows the accurate inclusion of quantum fluctuations due to nonlinear losses, which is a dominant effect when atom numbers are increased to improve fringe visibility.
Importantly, we can clearly demonstrate where fringe visibility is driven by quantum fluctuations, and where it is driven by trap inhomogeneity and dynamical effects, in order to choose optimal conditions for quantum noise reduction and spin squeezing. These calculations are a first step towards understanding mesoscopic superpositions and entanglement in ultracold atomic gases. An advantage of our method compared to the variational approaches used elsewhere Li et al. (2009); Sakmann et al. (2009) is that it allows us to treat a large number of independent field modes and particles, thus including degrees of freedom that are excited due to collisional and nonlinear loss dynamics Norrie et al. (2005); Deuar and Drummond (2007). Our theory can be readily extended to include finite temperature initial conditions Steel et al. (1998); Isella and Ruostekoski (2006), which will be treated elsewhere. Nonlinear losses and finite temperature effects can be also described within the confines of the variational approach Li et al. (2008); Sinatra et al. (2011).
Quantum phasediffusion is defined as the phase noise induced by number fluctuations which are conjugate to phase. This is a fundamental feature of BEC interferometry, and can only be removed when there are no interactions. However, there are other reasons for decoherence, which are also important. The approach used here captures all three significant features of atom interferometry that can result in decoherence: phasediffusion, losses, and trap inhomogeneity effects. The results given in this paper are applicable to simulations where the atom number per lattice point or mode is large. We focus on trapped BEC interferometry, for definiteness, although the method has a more general applicability.
We start by assuming that the BEC has wave interactions, together with Markovian losses due to body collisions. We employ a master equation together with the WignerMoyal quantum phasespace representation Gardiner and Zoller (2004) and a truncation of third and higherorder derivatives in the equations of motion. If we regard the commonly used GrossPitaevskii equation as a classical, first approximation to meanfield condensate dynamics, the truncated Wigner approach is best thought of as the second term in an expansion in inverse particle number. This truncation has been shown to be valid in the limit of large particle number Drummond and Hardman (1993); Steel et al. (1998); Sinatra et al. (2002). It has been further tested by comparison with the exact positiveP simulation method. The truncated Wigner method is particularly useful in lowdimensional and trap environments, where it has successfully predicted quantum squeezing and phasediffusion effects, in good agreement with dynamical experiments in photonic quantum soliton propagation Carter et al. (1987); Corney et al. (2008).
In the present Letter, we treat an ultracold, interacting multicomponent spinor Bose gas in effective dimensions. The basic Hamiltonian is easily expressed using quantum fields and , where creates a bosonic atom of spin at location , and destroys one; the commutators are The resulting physics of a dilute, lowtemperature Bose gas is welldescribed in the wave scattering limit by an effective Hamiltonian with contact interactions and external potentials:
(1) 
Here we omit the field argument for brevity, and use the Einstein summation convention of summing over repeated indices. is the singleparticle Hamiltonian:
(2) 
where is the atomic mass, is the external trapping potential for spin , is the internal energy of spin , represents a timedependent coupling that is used to rotate one spin projection into another, and is the atomatom interaction term. Thus, is the spin atomic density. For a dilute gas at low enough temperatures, , where is the wave scattering length in three dimensions. Here we assume a momentum cutoff , otherwise the couplings must be renormalized Sinatra et al. (2002).
We proceed by using a stochastic phasespace method that allows a numerical simulation of the quantum dynamics Drummond and Hardman (1993); Steel et al. (1998); Hoffmann et al. (2008). Defining a Wigner function , where is a cnumber field corresponding to the quantum field , this has a unitary timeevolution equation:
(3) 
Next, higher derivative terms of type are truncated. This approximation neglects higherorder terms in an expansion in , and is therefore valid in the limit of where is the atom number and is the number of lowenergy modes included Drummond and Hardman (1993); Sinatra et al. (2002); Norrie et al. (2006). In freespace calculations it is important to maintain this mode truncation. In the relevant limits where the technique is applicable, the equations simply reduce to GrossPitaevskii equations with Gaussian fluctuations of the initial conditions:
(4) 
For initial conditions in interferometry it is usually sufficient to consider a coherent state amplitude , corresponding to a typical initial state with Poissonian number fluctuations, as produced by a beamsplitter. In this case the initial Wigner amplitude has a Gaussian random distribution, with , where: This initial noise is necessary because the Wigner representation generates symmetrically ordered correlation functions, and includes vacuum fluctuations. For greater accuracy, the initial state can be modified to account for initial correlations, thermal noise, or additional fluctuations. If normal ordered correlations are measured, one has to express them as a sum of symmetrically ordered terms.
This includes all the known nonlinear quantum noise effects of quantum dynamics, like phase diffusion, entanglement and quantum squeezing, in the limit of large particle number. The initial noise terms do not occur in the semiclassical GrossPitaevskii approximation, which is therefore unable to predict these effects. Thus, while the lossless equations are identical to the GrossPitaevskii equations, the inclusion of initial noise terms together with nonlinear interactions leads to quantum phasediffusion. Such methods can be used for either freespace or trapped atom interferometry, provided there is an appropriate mode truncation.
Additional quantum noise enters from the effects of damping and losses, due to the fluctuationdissipation theorem. These effects are important at high densities in atomic traps. They can be included via an additional Markovian master equation Jack (2002) defined so that,
(5) 
where is the number of interacting particles, is a vector indicating the spins that are coupled, and we have introduced local Liouville loss terms,
(6) 
The reservoir coupling operators are the distinct fold products of local field annihilation operators, describing local body collision losses.
After transforming these new terms to evolution equations for the Wigner distribution, the drift term changes the GrossPitaevskii evolution to include nonlinear damping, while the next terms in the evolution equation give rise to additional FokkerPlanck diffusion terms associated with quantum noise from the loss reservoirs, given by:
(7) 
This leads to a stochastic equation:
(8) 
where the nonlinear loss has the form:
(9) 
and is a corresponding complex, stochastic deltacorrelated Gaussian noise with
(10) 
The multiplicative noise coefficient
(11) 
is a fluctuationdissipation term, so that the Wigner variables remain equivalent to the corresponding operators.
The loss coefficients in equations (8) can be converted to the conventional form, which is defined using atom number losses:
(12) 
where is the density of component and is the number of spin atoms lost in the collision. The conversion can be carried out as .
In this work we use a basis of plane waves in the volume , and the density of component is calculated as a probabilistic average:
(13) 
Here we use the fact that the approximate Wigner function is a probability distribution equivalent to an averaged sum over different simulation paths.

(a) 


(b) 

(c) 

(d) 
To illustrate the applications of this method we consider recent interferometry experiments with a twocomponent BEC involving two hyperfine states and in Rb Egorov et al. (2011). A conventional Ramsey sequence (Fig. 1, (a)) has been used with a BEC confined in a cigarshaped magnetic trap with the frequencies in a bias magnetic field of , so that magnetic field dephasing is largely eliminated Hall et al. (1998). The first pulse prepares a nonequilibrium superposition of states and and the spatial modes of two components periodically separate and merge again Mertes et al. (2007). The spatiallyseparated spin components evolve differently, as they have different scattering lengths. As a result, these collective oscillations lead to periodic dephasing and selfrephasing of the BEC components, clearly visible in both GPE and Wigner simulations of interference fringe visibility (Fig. 1, (b)). Asymmetric losses of two states are one cause of the contrast decay. This can be partially compensated by the application of a spin echo pulse midway through the evolution (Fig. 1, (c)). The GPE simulations wrongly predict (dashed lines) that visibility is largely recovered at long evolution times using the spin echo method. However, the addition of quantum noise (solid line) via the Wigner simulations noticeably speeds up the visibility decay even with a spin echo pulse present. This is in agreement with experimental observations, and shows that these effects play a significant part in the decay of visibility, even for large particle numbers.
The important feature of these quantum dynamical simulations is that they are able to treat large numbers of atoms (55,000 in this case), while correctly tracking all the quantum noise sources, and also extending the simulations to long timescales. Both of these features, large atom numbers and long timescales, are essential ingredients to accurate interferometric measurements. The simulations give accurate predictions despite large, multimode dynamical motion in three dimensions and substantial losses of most of the condensate atoms Egorov et al. (2011). On longer timescales, the experimental accuracy is limited by technical noises, and we have no data for comparisons.
The Wigner method is able to predict not only the average values of different observables, but their variances too. As an example, we now calculate the degree of squeezing , introduced in Wineland et al. (1994); Sørensen et al. (2001). This allows the analysis of experiments beyond the usual shot noise limit Riedel et al. (2010); Gross et al. (2010). If we define spin component operators as , and
(14) 
the average values of spin vector components can be calculated similarly to the average density in equation (13). Now we can shift the centre of coordinates to the end of the vector and rotate it, making the axis parallel to and choosing the remaining axes and so that is minimized.
Secondorder moments of spin operators are represented using fourthorder moments of field operators and, therefore, can be calculated using wavefunctions in Wigner representation. In this new coordinate system the squeezing parameter is expressed simply as
(15) 
where is the total number of atoms. The formula for the squeezing parameter in the original coordinate system can be found elsewhere Li et al. (2009). The squeezing parameter serves as a measure of atomic entanglement in the condensate, when the atoms are entangled if Sørensen et al. (2001).
As an illustration of the power of the Wigner method and of the effect of twobody losses we consider the temporal evolution of the squeezing parameter in a Ramsey interferometer for optically trapped twocomponent BEC in Rb (states and ) near a Feshbach resonance at (Fig. 2). Different intercomponent scattering lengths (corresponding to different magnetic fields) were used in order to find the optimal regime with significant squeezing. The value provides stronger nonlinear interactions, but larger twobody losses quickly eliminate the squeezing effect. Feshbach tuning to ensures the best squeezing ( at ), whereas long lasting squeezing is predicted for .
These simulations predict the degree of quantum noisereduction, which is a technique that can be used to improve precision quantum interferometry. The quantum noise is initially reduced due to a stretching and rotation of the quantum noise ellipse, similar to that found in quantum soliton squeezing Carter et al. (1987); Drummond et al. (1993). For lossless environments, this effect is optimized when the crossspecies scattering length is maximally different to the intraspecies scattering length, which is found near the Feshbach resonance. However, there are competing nonlinear loss effects at the Feshbach resonance, which means that some detuning of the magnetic field is essential to reduce these detrimental losses. Subsequently, the squeezing is destroyed in time as the two fields recombine and interfere with each other. Importantly, these quantum squeezing calculations indicate conditions that will allow this macroscopic quantum effect to be experimentally observed in ultracold atomic BEC for much larger atom numbers than calculated previously.
In conclusion, the truncated WignerMoyal quantum phasespace theory is wellsuited for a variety of calculations of manybody dynamics of quantum degenerate gases. Although the Wigner function is not a true probability, it becomes one to a good approximation in the limit of large particle number, so that a probabilistic (random) sampling of phasespace trajectories can be used to treat quantum fluctuations. Furthermore, it is straightforward to treat a spatially inhomogeneous, manymode problem as found in an extended 3dimensional environment. Initial conditions such as a coherent beamsplitter as employed in typical atom interferometry experiments can be readily included, with proper accounting for both quantum effects and nonlinear losses in the condensate.
References
 P. D. Drummond and A. D. Hardman, Europhys. Lett. 21, 279 (1993).
 M. Steel et al., Phys. Rev. A 58, 4824 (1998).
 A. Sinatra, C. Lobo, and Y. Castin, J. Phys. B 35, 3599 (2002).
 Y. Li et al., Eur. Phys. J. B 68, 365 (2009).
 K. Sakmann et al., Phys. Rev. Lett. 103, 220601 (2009).
 A. Norrie, R. Ballagh, and C. Gardiner, Phys. Rev. Lett. 94, 040401 (2005).
 P. Deuar and P. Drummond, Phys. Rev. Lett. 98, 120402 (2007).
 L. Isella and J. Ruostekoski, Phys. Rev. A 74, 063625 (2006).
 Y. Li, Y. Castin, and A. Sinatra, Phys. Rev. Lett. 100, 210401 (2008).
 A. Sinatra et al., Phys. Rev. Lett. 107, 060404 (2011).
 C. Gardiner and P. Zoller, Quantum Noise, 4th ed. (Springer, 2004) p. 449.
 S. J. Carter et al., Phys. Rev. Lett. 58, 1841 (1987).
 J. Corney et al., Phys. Rev. A 78, 023831 (2008).
 S. Hoffmann, J. Corney, and P. D. Drummond, Phys. Rev. A 78, 013622 (2008).
 A. Norrie, R. Ballagh, and C. Gardiner, Phys. Rev. A 73, 043617 (2006).
 M. Jack, Phys. Rev. Lett. 89, 140402 (2002).
 M. Egorov et al., Phys. Rev. A 84, 021605(R) (2011).
 K. Mertes et al., Phys. Rev. Lett. 99, 190402 (2007).
 D. Hall et al., Phys. Rev. Lett. 81, 4532 (1998).
 A. Kaufman et al., Phys. Rev. A 80, 050701 (2009).
 D. Wineland et al., Phys. Rev. A 50, 67 (1994).
 A. Sørensen et al., Nature 409, 63 (2001).
 M. F. Riedel et al., Nature 464, 1170 (2010).
 C. Gross et al., Nature 464, 1165 (2010).
 P. D. Drummond et al., Nature 365, 307 (1993).