# Fast generation of -atom Greenberger-Horne-Zeilinger state in separate coupled cavities via transitionless quantum driving

## Abstract

By jointly using quantum Zeno dynamics and the approach of “transitionless quantum driving (TQD)” proposed by Berry to construct shortcuts to adiabatic passage (STAP), we propose an efficient scheme to fast generate multiatom Greenberger-Horne-Zeilinger (GHZ) states in separate cavities connected by opitical fibers only by one-step manipulation. We first detail the generation of the three-atom GHZ states via TQD, then, we compare the proposed TQD scheme with the traditional ones with adiabatic passage. At last, the influence of various decoherence factors, such as spontaneous emission, cavity decay and fiber photon leakage, is discussed by numerical simulations. All the results show that the present TQD scheme is fast and insensitive to atomic spontaneous emission and fiber photon leakage. Furthermore, the scheme can be directly generalized to realize -atom GHZ states generation by the same principle in theory.

###### pacs:

03.67. Pp, 03.67. Mn, 03.67. HK## I Introduction

Quantum entanglement is not only one of the most important features in quantum mechanics (1), but also a key resource for testing quantum mechanics against local hidden theory (2). Recently, the entangled states have been applied in many fields in quantum information processing (QIP), such as quantum computing (3), quantum cryptography (4), quantum teleportation (5); (6), quantum secret sharing (7), and so on. These promising applications have greatly motivated the researches in the generation of entangled states.

It is worth noting that a typical entangled state so-called
Greenberger-Horne-Zeilinger (GHZ) state
, first
proposed and named by Daniel M. Greenberger, Machael Horne and Anton
Zeilinger (8), has raised much interest. Contrary to
other entangled states, the GHZ state exhibits some special
features, such as it is the maximally entangled state and can
maximally violate the Bell inequalities (9). In 2001,
Zheng has proposed a scheme to test quantum mechanics against local
hidden theory without the Bell’s inequalities by use of multiatom
GHZ state (10). Therefore, great interest has arisen
regarding the significant role of GHZ state in the foundations of
quantum mechanics measurement theory and quantum communication. At
present, the first and main problem we face is how to generate GHZ
state by using current technologies. To our knowledge, in some
experimental systems, such as trapped ions systems (11),
photons systems (12); (13), and atoms systems
(14), scientists have realized the generation of such
GHZ state. Recently, a promising experimental instrument named
cavity quantum electrodynamics (C-QED), which concerns the
interaction between the atom and the quantized field within cavity
(15), has aroused much attention. Based on C-QED,
many theoretical schemes for generating GHZ state have been
proposed. For example, Li *et al.* have proposed a scheme to
generate multiatom GHZ state under the resonant condition by Zeno
dynamics (16), but the scheme is sensitive to the atomic
spontaneous emission and fiber photonic leakage. Hao *et al.*
have proposed an efficient scheme to generate mulitiatom GHZ state
under the resonant condition via adiabatic passage
(17), but it takes too long time. Chen *et al.*
have proposed a smart scheme to overcome the above drawbacks, but
the scheme needs to trap three atoms in one cavity
(18), such design is difficult to manipulate each
atom in experiment and to construct a large-scale quantum network.

On the other hand, in modern quantum application field, an important method to manipulate the states of a quantum system is adiabatic passage, included “rapid” adiabatic passage (RAP), stimulated Raman adiabatic passage (STIRAP), and their variants (19). The adiabatic passage covers the shortage with respect to errors or fluctuations of the parameters compared with the resonant pulses, but its evolution speed is very slow, so it may be useless in some cases. In recent years, shortcuts to adiabatic passage (STAP), which accelerates a slow adiabatic quantum process via a non-adiabatic route, has aroused a great deal of attention. Many theoretical proposals have been presented to realize QIP, such as fast population transfer (20); (21); (22); (23), fast entanglement generation (22); (24), fast implementation of quantum phase gates (25); (26), and so on. To our knowledge, the main methods to construct effective shortcuts has two forms: one is invariant-based inverse engineering based Lewis-Riesenfeld invariant (IBLR) (27) and the other is transitionless quantum driving (TQD) (28), which is pointed out by Berry. The two methods are strongly related (29), but also have their own characteristics. For example, the former does not need to modify the original Hamiltonian , but the algorithm is suitable for some special physical models. The latter needs to modify the original Hamiltonian to the “counter-diabatic driving” (CDD) Hamiltonian to speed up the quantum process. The fixed Hamiltonian can be obtained in theory, but it does not usually exist in real experiment.

In addition, the quantum Zeno effect (QZE), first understood by Neumann (30) and named by Misra and Sudarshan (31), exhibits a especially experimental phenomenon that transitions between quantum states can be hindered by frequent measurement. The system will evolve away from its initial state and remain in the so-called “Zeno subspace” defined by the measure due to frequently projecting onto a multi-dimensional subspace (32); (33). This is so-called quantum Zeno dynamics (QZD). Without making using of projection operators and non-unitary, “a continuous coupling” can obtain the same quantum Zeno effect instead of discontinuous measurements (34); (35). Now, we give a brief introduction of the quantum Zeno dynamics in the form of continuous coupling (35). Suppose that the system and its continuously coupling external system are governed by the total Hamiltonian , where is the Hamiltonian of the quantum system to be investigated, is an additional Hamiltonian caused by the interaction with the external system, is the coupling constant. In the limit , the evolution operator of system can be expressed as , where is the eigenprojection of corresponding to the eigenvalue , i.e., (36).

Inspired by the above useful works, we make use of Zeno dynamics and TQD to construct STAP to generate -atom GHZ state in C-QED. Our scheme has the following advantages: (1) The atoms are trapped in different cavities so that the single qubit manipulation is more available in experiment. (2) The fast quantum entangled state generation for multiparticle in spatially separated atoms can be achieved in one step. (3) Numerical results show that our scheme is not only fast, but also robust against variations in the experimental parameters and decoherence caused by atomic spontaneous emission and fiber photon leakage. In fact, further research shows that, the total operation time for the scheme is irrelevant to the number of qubits.

The paper is organized as follows. In section II, we give a brief introduction to the approach of TQD proposed by Berry. In section III, we introduce the physical modal and the systematic approximation by QZD. In section IV, we propose the schemes to generate the three-atom GHZ state via TQD and adiabatic passage, respectively. The decoherence caused by various factors is discussed by the numerical simulation. In section V, we directly generalize the scheme in section IV to generate -atom GHZ states in one step. At last, we discuss the experimental feasibility and make a conclusion about the scheme in section VI.

## Ii Transitionless quantum driving

Suppose a system is dominated by a time-dependent Hamiltonian with instantaneous eigenvectors and eigenvalues ,

(1) |

When a slow change satisfying the adiabatic condition does, the system governed by can be expressed at time

(3) | |||||

(4) |

where . Because the instantaneous eigenstates do not meet the Schrdinger equation , a finite probability that the system is in the state will occur during the whole evolution process even under the adiabatic condition.

To construct the Hamiltonian that drives the instantaneous eigenvector exactly, i.e., there are no transitions between different eigenvectors during the whole evolution process, we define the unitary operator

(5) |

we can formally solve the Schrödinger equation

(6) |

Substituting eq. (3) into eq.(4), the Hamiltonian can be expressed

(7) |

the simplest choice is , for which the bare states , with no phase factors, are driven by

(8) |

## Iii Physical modal and systematic approximation by QZD

For the sake of the clearness, let us first consider the physical modal that three identical atoms , and are trapped in three linearly arranged optical cavities , and , respectively. As shown in FIG. 1, each atom possesses one excited level and three ground states , and . The cavities and are single-mode, the cavity are bi-mode. , and are connected by the optical fibers , , respectively. Assuming that the transition is resonantly driven by a external classical field with the time-dependent Rabi frequencie , while the transition is resonantly coupled to the left-circularly(right-circularly) polarized cavity mode with the coupling constant , respectively.

In the short-fiber limit, i.e., ( is the length of the fibers, is the decay rate of the cavity fields into a continuum of fiber modes and is the speed of light), only one resonant mode of the fiber interacts with the cavity mode (37). In the rotating frame, the Hamiltonian of the whole system can be written as

(10) | |||||

(12) | |||||

(15) | |||||

where and denote the creation and annihilation operators for the left-circularly (right-circularly) polarized mode of cavities , respectively; and denote the creation and annihilation operators associated with the resonant mode of fiber , respectively. For the sake of simplicity, we assume and . If the initial state of the whole system is (here ), the whole system evolves in the following subspaces

(17) | |||||

(19) | |||||

(21) | |||||

(23) | |||||

(25) | |||||

(26) |

where denotes the state of the atoms in every cavity, means that the quantum field state of system contains photons. means that the number of left-circularly photon is and the number of right-circularly photon is in the cavity .

Under the Zeno condition , the Hilbert subspace is split into nine invariant Zeno subspace

(28) | |||||

(30) | |||||

(31) |

where the eigenstates of are

(33) | |||||

(35) | |||||

(37) | |||||

(39) | |||||

(41) | |||||

(43) | |||||

(45) | |||||

(47) | |||||

(48) |

with the corresponding eigenvalues

(50) | |||||

(52) | |||||

(53) |

where the parameters are

(55) | |||||

(57) | |||||

(59) | |||||

(60) |

in addition, and is the normalization factor of the eigenstate .

The projector in the th Zeno subspace is

(61) |

The Hamiltonian in Eq. (8) can be approximately given by

(63) | |||||

(64) |

If the initial state is , it reduces to

(65) |

which can be treated as a simple three-level system with an excited state and two ground states and . Then we obtain the eigenvectors and eigenvalues of the effective Hamiltonian as

(66) |

with the corresponding eigenvalues and , and and .

## Iv The generation of the three-atom GHZ state via transitionless quantum driving and adiabatic passage

### iv.1 Adiabatic passage method

For the sake of the clearness, we first briefly present how to generate the three-atom GHZ state via adiabatic passage. When the adiabatic condition is fulfilled well and the initial state is , the state evolution will always follow closely. To generate the three-atom GHZ states via the adiabatic passage and meet the boundary conditions of the fractional stimulated Raman adiabatic passage (STIRAP),

(67) |

we need properly to tailor the Rabi frequencies and in the original Hamiltonian

(69) | |||||

(70) |

where is the pulse amplitude and is the operation time. and are some related parameters to be chosen for the best performance of the adiabatic passage process. In order to achieve better performance and meet the boundary conditions, we suitably chose the parameters that , and . As shown in Fig. 2, the time-dependent and versus are plotted with the fixed values and . With the above parameters, we obtain our wanted three-atom GHZ state via the adiabatic passage. But this evolution process needs a relatively long time to satisfy the adiabatic condition. We will detail the reasons in the section of numerical simulations and analyses.

### iv.2 Transitionless quantum driving method

To reduce the evolution time and obtain the same state as the adiabatic passage, we use the approach of TQD to construct STAP. As introduced in the above, STAP speeds up a slow adiabatic passage via a non-adiabatic passage route to achieve a same outcome, and the TQD method is a important route to construct shortcuts. According to the ideas proposed by Berry (28), the instantaneous states in Eq. (16) do not meet the Schrödinger equation, i.e., , so the situation that the system starts from the state and ends up in the state occurs in a finite probability even under the adiabatic condition. To drive the instantaneous states exactly, we look for a Hamiltonian related to the original Hamiltonian according to Berry’s transitionless tracking algorithm (28). From section II, we know the simplest Hamiltonian possessed the form,

(71) |

Substituting Eq. (16) in Eq. (19), we obtain

(72) |

where . This is our wanted CCD Hamiltonian to construct STAP, and we will detail how to construct this Hamiltonian in experiment later.

For the present system, the CDD Hamiltonian is given in Eq. (18), but it is irrealizable under current experimental condition. Inspired by Refs. [17, 19], we find an alternative physically feasible (APF) Hamiltonian whose effect is equivalent to . The design is shown in Fig. 3, the atomic transitions is not resonantly coupled to the classical lasers and cavity modes with the detuning . The Hamiltonian of the system reads , where . Then, similar to the approximation by QZD in section III, we also obtain an effective Hamiltonian for the non-resonant system

(73) |

When the large detuning condition is satisfied, we can adiabatically eliminate the state and obtain the final effective Hamiltonian

(74) |

For simplicity, we set . The front two terms caused by Stark shift can be removed and the Hamiltonian becomes

(75) |

where . The equation has a similar form with Eq. (20), but the effective couplings between and exist -dephased. To guarantee their consistency, we put a change that . Then, the eigenstates of become

(76) |

and the CDD Hamiltonian becomes

(77) |

Compared Eq. (23) with Eq. (25), we can easily get the CDD Hamiltonian when the condition is satisfied.

(78) |

### iv.3 Numerical simulations and analyses

Next we will show that it takes less time to get the target state on the situation governed by the APF Hamiltonian via TQD than by the original Hamiltonian via adiabatic passage. The time-dependent population for any state is defined as , where is the corresponding time-dependent density operator. We present the fidelity versus the laser pulses amplitude and the operation time via adiabatic passage in Fig. 4. As shown in Fig. 4, we can know that the bigger the laser pulse amplitude is, the less time that the system evolution to the target state needs. However, we need to satisfy the Zeno conditions , so we set . In Fig. 5, we display the time-dependent populations of the states , , and via adiabatic passage. As depicted in Fig. 4 and Figs. 5, the operation time needs to achieve an ideal result at least. It is awkward in some case.

Next we will detail the evolution governed by the APF Hamiltonian via TQD. According to eq. (24) we finally get a GHZ state . In Fig. 6, we present the relationship between the fidelity of the three-atom GHZ state (governed by the APF Hamiltonian) and two parameters and when to satisfy the Zeno condition, where the fidelity of the three-atom GHZ state is defined as ( is the desity operator of the whole system when ). We find that a wide range for parameters and can obtain a high fidelity of the three-atom GHZ state, and the fidelity increases with the increasing of and the decreasing of . In order to satisfy the large detuning condition, we set . The Fig. 6 reveals that the operation time needs via TQD at least. In Figs. 7 we plot the operation time for the creation of the GHZ state governed by and by with the parameters that , , and . Numerical results show that the APF Hamiltonian can govern the evolution to a perfect GHZ state from in a relatively short interaction time while the original Hamiltonian can not.

In above analysis, we do not consider the influence of decoherence caused by various factors, such as spontaneous emissions, cavity decays and fiber photon leakages. In fact, the decoherence is unavoidable during the evolution of the whole system in experiment. The master equation of the whole system is written as

(87) | |||||

where is the atomic spontaneous emission rate for the th atom and is the decay rate of the th cavity (th fiber), denotes the atomic transition from the ground states to the excited state . For the sake of simplicity, we assume that , and . As shown in Fig. 8, we plot the fidelity governed by the APF Hamiltonian and by the original Hamiltonian