# Interference of spin-orbit coupled Bose-Einstein condensates.

## Abstract

Interference of atomic Bose-Einstein condensates, observed in free expansion experiments, is a basic characteristic of their quantum nature. The ability to produce synthetic spin-orbit coupling in Bose-Einstein condensates has recently opened a new research field. Here we theoretically describe interference of two noninteracting spin-orbit coupled Bose-Einstein condensates in an external synthetic magnetic field. We demonstrate that the spin-orbit and the Zeeman couplings strongly influence the interference pattern determined by the angle between the spins of the condensates, as can be seen in time-of-flight experiments. We show that a quantum backflow, being a subtle feature of the interference, is, nevertheless, robust against the spin-orbit coupling and applied synthetic magnetic field.

###### pacs:

03.75.-b###### pacs:

42.25.Hz###### pacs:

71.70.Ej###### pacs:

75.70.TjMatter waves Interference Spin-orbit coupling, Zeeman and Stark splitting, Jahn-Teller effect Spin-orbit effects

## 1 I. Introduction

Interference of matter waves is one of the most interesting effects in quantum physics. The interference of two expanding Bose-Einstein condensates is a clear manifestation of quantumness in macroscopic systems [2, 3, 4]. It can be observed by preparing two condensates in spatially separated harmonic traps, that are released afterwards. Then, the condensates can expand freely and eventually overlap, producing an interference pattern.

The quantum dynamics becomes much richer for spin-orbit coupled Bose-Einstein condensates, where optically produced pseudospin is coupled to the atomic momentum and to a synthetic, also optically produced, magnetic field [5, 6, 7]. These effects, which open a venue to the simultaneous control of orbital and spin degrees of freedom and to experimental observation of new phases and dynamic processes have been discussed for a variety of ultracold atomic systems [8, 9, 10, 11, 12, 13, 14, 15, 17, 16, 18] including recently produced and studied Fermi gases with synthetic spin-orbit coupling [19, 20]. In quantum information technologies, spin-orbit coupled Bose-Einstein condensates can serve as a realization of macroscopic qubits, as proposed in [11]. State-of-the-art reviews can be found in [21, 22].

Here we consider time-of-flight control of interference of two spin-orbit- and Zeeman-coupled one-dimensional condensates (as shown in Fig.1) producing their entangled state, which might be required for quantum information purposes [11]. The condensates, that move freely in a waveguide realized by tight confinement in the transverse directions, give rise to an interference pattern that strongly depends on the relative orientation of their pseudospins. We study the role of the synthetic magnetic field on the interference and show that it can be fully controlled by changing the synthetic Zeeman coupling. In addition, we show that the quantum backflow [23, 24, 25, 26, 27, 28, 29, 30], being a subtle effect of the interference, is rather robust against mutual orientation of spins of the condensates.

## 2 II. Interference of condensates with spin-orbit and Zeeman coupling

To study the spin-dependent interference of two condensates, we take the synthetic magnetic field along the -axis and spin-orbit coupling field along the - axis. The Hamiltonian becomes:

(1) |

where is the momentum operator, is the particle mass, is the spin-orbit coupling constant, and are the Pauli matrices, and is the Zeeman splitting. To see the qualitative effect of the spin-orbit coupling, we begin with a single packet where the solution of the Schrödinger equation

(2) |

is

(3) |

Here , is the wave function in the momentum space, and is the initial spinor normalized with . We assume without loss of generality that and are real. For definiteness, we take Gaussian , produced by an initial state in a harmonic trap, as described in Ref.[30]. This function is given by:

(4) |

where is the mean momentum, is the initial width, and is the initial position.

For a packet narrow in the momentum space with one can neglect momentum distribution and write the wavefunction (3) as a product where is the time and coordinate dependence in the absence of spin-orbit coupling. The spin state of a packet is given by:

(5) |

where is the mean value of a spin contribution to the Hamiltonian (1). We use Eq.(5) below for a qualitative analysis of the packets’ interference.

As a result, the spin of a wavepacket with well-defined momentum rotates around the axis (cf. Fig.1):

(6) |

with the rate

(7) |

where Figure 1 shows rotating spins in the presence of Zeeman splitting and directions of the vectors in (6), where index labels the condensate, and we use for corresponding mean values.

If , the spinor components in (3) are decoupled and have the form:

(8) |

where The -determined phase shift between and in (8) leads to a coordinate-dependent spin rotation. The same results for spin motion can be obtained by gauging out the spin-orbit coupling in Eq.(1) by a coordinate-dependent spin rotation ( is the spin rotation length), calculating the resulting dynamics, and then making the inverse transformation to obtain the observables [31, 32]. However, in the presence of a Zeeman field, which is of our interest, gauging out the spin-orbit coupling leads to a coordinate-dependent effective magnetic field. Although transport effects can be obtained with Eq.(5) (see, e.g [33]), general dynamics is difficult to treat beyond perturbation theory [34]. For this reason we use the direct calculation rather than the spin rotation approach.

The expectation values of the packet width and velocity at time obtained with Eq.(8) are

(9) |

(10) |

Here .

For a general form of the current density is given by:

(11) |

where The experimentally measured density is related to by the continuity equation. For the weak coupling considered below we neglect the -related terms in Eqs.(9)-(11).

To see the effect of the spin-orbit coupling on interference of condensates, we take the initial wave function in the form where the coherence can be achieved, e.g. by a technique proposed in [2]:

(12) |

Here the amplitudes and are normalized as is the corresponding spinor, and is defined by (4). The average velocities of the packets are determined by (10) for the corresponding momentum and spin state, and from now on we omit in the notation of averages. Using (3) and (12) we obtain the exact evolution of two initial wave packets with spin-orbit coupling.

For a qualitative understanding we use a model of two independent condensates moving with different momenta. Take first as an illustration a system with the following :

(13) |

where

(14) |

The current density (11) for the wave function (13) is defined by:

(15) | |||||

where and . Equation (15) shows that the interference, seen here as the fast oscillations in the coordinate or time-dependence of the current, is controlled by the spin states through the product

General expressions for are cumbersome. Taking as an example packets with well-defined momenta and spins initially parallel to the -axis, we find with (5):

(16) |

where and are defined by (7). If we obtain , with the angle

(17) |

Equation (16) shows how the mutual orientation of the spins of the condensates and, in turn, their interference, depends on the time of flight in the presence of spin-orbit or Zeeman coupling. In particular, if at the spin states are orthogonal, the interference disappears, which shows that it can be controlled by manipulating the condensate spin.

Let us now consider specific examples for . We use in numerical calculations the system of units with , mass , unit length of one micron, and dimensionless parameters:

(18) |

corresponding to both condensates with the spin oriented along the -axis. We take time-of-flight and the wave packet “collision” point at . To make connection with possible experimental observations, we take atom as an example. The resulting velocity unit is 0.072 cm/s and, therefore, the unit of time is approximately s. As a result, corresponds to about 28 milliseconds and the initial distance between the packets (for and ) of 120 microns. Below we consider two realizations of the condensates, with equal and different widths.

First, we take both initial widths equal, . At the meeting time , if the spin states of the condensates are orthogonal, that is the interference is destroyed. For , we obtain the constructive (destructive) interference with similar fringes, just shifted by half period. Here the interference is maximal and, for the same as in the absence of spin-related effects. We take spin-orbit coupling corresponding to the two realizations of the angle between the spins of condensates at the collision point (see (17)):

(19) | |||

(20) |

respectively.

In Fig. 2 one can see that, for there is no interference in the flux, while for the flux is characterized by a strong interference pattern and by the presence of backflow, namely a negative current density, , see Fig. 2 [23, 24, 25, 26, 27, 28, 29, 30]. For other values of spin-orbit coupling the flux interference is between these two limits.

2. For different initial widths of the packets at the time-of-flight the spreads of the packets can be, in general, different. The same holds for the travel time of the packets through the point defined as

(21) |

where and are the velocities of the packets determined in (10), and are the widths of the packets at the meeting time determined in (9), and we have taken into account that the traveling time of wave function is of the order of .

In this case, the duration of the interference (interference time) is

(22) |

If the coupling is large, the spins of the packets rotate fast and during the time interval the interference would be destroyed several times depending on the rotation rate. Then the number of points in time domain where the interference disappears can be estimated as:

(25) |

In this formula the factor 2 means that, in one period of rotation of the angle between spins, the interference is destroyed twice when spin states are orthogonal. In addition, if the packets are initially narrow, and, therefore, spread with a large rate of the order of , one can see the effect of multiple interferences better. From Fig. 3 one can see that, during the interference time the spin states become orthogonal once, and the interference is destroyed at this instant.

Below we consider the effects of the Zeeman term limiting ourselves to equal initial widths of the packets with all other initial parameters (18) unchanged. It is important here that if the condition is satisfied, the vectors (6) are very close to each other and to the -axis, and the spins be always parallel to each other with a high accuracy. Fig. 4 demonstrates the spin states (16) and shows that the expression (16) is zero only when . As a result with synthetic magnetic field the interference cannot be completely destroyed by spin-orbit coupling.

Now we evaluate the effect of on the time-dependent flux as a function of the Zeeman coupling. For this purpose we use the Fourier series in the time domain and define:

(26) |

with the coefficients

(27) |

where is the full collision time interval. For summation limit the function (26) is in (11). To quantitatively describe the interference, first we filter out high-frequency Fourier components from the time dependence by taking a smaller (in our case ) limit in Eq.(26). Now, the high-frequency terms do not contribute, and in Fig. 6 we see that plot of the function (11) symmetrically oscillates around the plot of the filtered function (26). The maximal amplitude of oscillation is obtained for and . As a result, one can define the value corresponding to the strongest interference as:

(28) |

having the value of at given system parameters. The efficiency of the interference as a function of is characterized by:

(29) |

and the contribution of the backflow is evaluated as:

(30) |

The evaluation of interference and backflow, (29) and (30) dependent on is plotted in Fig. 5 for given values of spin-orbit coupling (19) and (20). Fig. 5 and 6 show that it is possible to control the interference of two condensates using the spin-orbit coupling and synthetic magnetic field. For strong field spins of particles are frozen in one direction and interference is maximal. The zero value of the function corresponds to the absence of backflow, where the flux for any . As one can see, the intervals of its zero values are relatively small, meaning that the backflow is robust against the spin-dependent interactions. Figure 5 shows that for the given system parameters the backflow disappears if the interference parameter is less than 0.5.

As for the role of the interactions, they do not influence the momentum of the packet, so they do not change its mean spin precession rate, affecting the spins only marginally. However they do influence the packet width and can prevent collision if they are strong enough. To avoid these effects in the regime and it is sufficient to satisfy the condition of small contribution of the interatomic repulsion into the packet width. Since in the absence of repulsion the packet spreads with the rate of the order of , the interaction energy per atom should be less than to satisfy this condition. A good candidate for a very weakly interacting BEC is ensemble, although, to the best of our knowledge, spin-orbit coupling effects have not been reported for this isotope.

## 3 III. Conclusions

We have shown that the superposition of two freely moving spin-orbit coupled condensates gives rise to interference effects strongly dependent on the spin state of the condensates at the collision time. The interference - characterizing both the density and the flux - is strong when the spins of the two condensates are parallel, and it disappears when the spin states are orthogonal. These effects can be clearly seen in time-of-flight experiments, and are at reach with the current technology for ultracold atoms. In addition, the system exhibits a spin-dependent quantum backflow behavior, which is relatively robust against synthetic spin-orbit coupling and magnetic field. The ability to control the interference by synthetic spin-orbit coupling and magnetic field can be useful for investigating the quantum properties of atomic condensates and for interference of macroscopic spin-orbit coupled BEC-based qubits for quantum information applications.

###### Acknowledgements.

This work was supported by the University of Basque Country UPV/EHU under program UFI 11/55, Spanish MEC (FIS2012-36673-C03-01 and FIS2012-36673-C03-03), and Grupos Consolidados UPV/EHU del Gobierno Vasco (IT-472-10). S.M. acknowledges EU-funded Erasmus Mundus Action 2 eASTANA, ”evroAsian Starter for the Technical Academic Programme” (Agreement No. 2001-2571/001-001-EMA2). M.P. is supported by the Doctoral Scholarship of the University of Basque Country UPV/EHU.### References

- \NameCastin Y. Dalibard J. \REVIEWPhys. Rev. A5519974330.
- \NameAndrews M. R., Townsend C. G., Miesner H.-J., Durfee D. S., Kurn D. M. Ketterle W. \REVIEWScience2751997637.
- \NameBand Y. B. \REVIEWJ. Phys. Chem. B112200816097.
- \NameLin Y.-J., Compton R. L., Jiménez-Garcia K., Porto J. V. Spielman I. B. \REVIEWNature4622009628.
- \NameWang C., Gao C., Jian C.-M. Zhai H. \REVIEWPhys. Rev. Lett.1052010160403
- \NameLin Y.-J., Jiménez-García K. Spielman I. B. \REVIEWNature471201183.
- \NameDudarev A. M., Diener R. B., Carusotto I. Niu Q. \REVIEWPhys. Rev. Lett.922004153005.
- \NameOsterloh K., Baig M., Santos L., Zoller P. Lewenstein M. \REVIEWPhys. Rev. Lett.952005010403
- \NameRuseckas J., Juzeliūnas G., Öhberg P. Fleischhauer M. \REVIEWPhys. Rev. Lett.952005010404.
- \NameStanescu T. D., Anderson B. Galitski V. \REVIEWPhys. Rev. A782008023616.
- \NameLiu X.-J., Borunda M. F., Liu X. Sinova J. \REVIEWPhys. Rev. Lett.1022009046402.
- \NameJuzeliūnas G., Ruseckas J. Dalibard J. \REVIEWPhys. Rev. A.812010053403.
- \NameHo T.-L. Zhang S. \REVIEWPhys. Rev. Lett.1072011150403
- \NameLi Y., Martone G. Stringari S. \REVIEWEPL 99 2012 56008; \NameMartone G.I., Li Y., Pitaevskii L.P. Stringari S. \REVIEWPhys. Rev. A 86 2012 063621.
- \NameZhang J.-Y. et al. \REVIEWPhys. Rev. Lett.1092012115301
- \NameAnderson B. M., Juzeliūnas G., Galitski V. M. Spielman I. B. \REVIEWPhys. Rev. Lett.1082012235301.
- \NameZhang Y., Mao L., Zhang Ch. \REVIEWPhys. Rev. Lett.1082012035302.
- \NameWang P. et al. \REVIEWPhys. Rev. Lett.1092012095301.
- \NameCheuk L. W. et al. \REVIEWPhys. Rev. Lett.1092012095302.
- \NameZhai H. \REVIEWInt. J. Mod. Phys. B 26 2012 1230001.
- \NameGalitski V. Spielman I. B. \REVIEWNature494201349.
- \NameAllckok G. R. \REVIEWAnn. Phys. (NY)531969253, 286, 311.
- \NameBracken A. J. Melloy G. F. \REVIEWJ. Phys. A: Math. Gen2719942197.
- \NameMuga J. G., Palao J. P. Sala R. \REVIEWPhys. Lett. A238199890.
- \NameMuga J. G. Leavens C. R. \REVIEWPhys. Rep.3382000353.
- \NameDamborenea J. A., Egusquiza I. L., Hegerfeldt G. C. Muga J. G. \REVIEWPhys. Rev. A662002052104.
- \NameBerry M. V. \REVIEWJ. Phys. A: Math. Theor.432010415302.
- \NameYersley J. M., Halliwell J. J., Hartshorn R. Whitby A. \REVIEWPhys. Rev. A862012042116.
- \NamePalmero M., Torrontegui E., Muga J. G. Modugno M. \REVIEWPhys. Rev. A872013053618.
- \NameTokatly I. V. Sherman E. Ya. \REVIEWPhys. Rev. B822010161305.
- \NameGlazov M. M. Sherman E. Ya. \REVIEWPhys. Rev. Lett.1072011156602.
- \NamePershin Yu. V, Nesteroff J. A. Privman V. \REVIEWPhys. Rev. B692004121306(R).
- \NameLevitov L. S. Rashba E. I. \REVIEWPhys. Rev. B672003115324.