Quantum Fuel with Multilevel Atomic Coherence for
Ultrahigh Specific Work in a Photonic Carnot Engine
We investigate scaling of work and efficiency of a photonic Carnot engine with the number of quantum coherent resources. Specifically, we consider a generalization of the “phaseonium fuel” for the photonic Carnot engine, which was first introduced as a three-level atom with two lower states in a quantum coherent superposition by [M. O. Scully, M. Suhail Zubairy, G. S. Agarwal, and H. Walther, Science 299, 862 (2003)], to the case of level atoms with coherent lower levels. We take into account atomic relaxation and dephasing as well as the cavity loss and derive a coarse grained master equation to evaluate the work and efficiency, analytically. Analytical results are verified by microscopic numerical examination of the thermalization dynamics. We find that efficiency and work scale quadratically with the number of quantum coherent levels. Quantum coherence boost to the specific energy (work output per unit mass of the resource) is a profound fundamental difference of quantum fuel from classical resources. We consider typical modern resonator set ups and conclude that multilevel phaseonium fuel can be utilized to overcome the decoherence in available systems. Preparation of the atomic coherences and the associated cost of coherence are analyzed and the engine operation within the bounds of the second law is verified. Our results bring the photonic Carnot engines much closer to the capabilities of current resonator technologies.
A practical figure of merit to compare fuel and battery materials is the specific energy, or energy to mass ratio Chalk and Miller (2006); Chau et al. (1999); Yang et al. (2010). As a material constant, it measures the energy that will be harvested by using a unit mass of the material. About a decade ago, a highly non-traditional fuel, called “phaseonium”, which is a three level atom with two lower states in a quantum coherent superposition, was proposed to be used in a Photonic Carnot engine (PCE) Scully et al. (2003). Phaseonium engine could work with a single heat bath and a phaseonium reservoir Scully et al. (2003); Scully (2002); Rostovtsev et al. (2003); Zubairy (2002). This proposal stimulated much interest to quantum heat engines Kieu (2004); Quan et al. (2007); Allahverdyan et al. (2008); Johal (2009); Wang et al. (2012); Dorfman et al. (2013); Li et al. (2013); Zhuang and Liang (2014); Altıntaş et al. (2014, 2015); Uzdin et al. (2015); Niedenzu et al. (2015); Hardal and Müstecaplıoğlu (2015). It was later argued that existing resonator systems can not implement such an engine, due to high cavity losses and atomic dephasing Quan et al. (2006). Here, we address a fundamental question of how the specific energy of phaseonium fuel is scaled with the number of quantum coherent levels. A favorable scaling law against decoherence and dephasing could bring the phaseonium engine closer to available practical systems.
We describe multilevel generalization of phaseonium fuel in Fig. 1. The block diagonal density matrix of an level atom is shown in Fig. 1(a). The excited level, denoted by Â“”, and the lower levels, denoted by “” are well separated from each other by an energy measured from the central lower level as shown in Fig. 1(b). The lower levels can be degenerate or non-degenerate. The diagonal elements , and , with , determine the level populations, while the off diagonal elements , with , indicate the coherence between the levels. Coherence can be characterized by the magnitude and phase of the complex number .
Though both the amplitude and the phase of coherent superposition states can be controlled in experiments Vewinger et al. (2007), the main control variable for the photonic Carnot engine is the phase of the coherence as the amplitude is required to be small enough to keep the system only slightly out of thermal equilibrium. The complete graphs in Fig. 1(a) have nodes and links, representing the atomic energy levels and the coherences between them, respectively. The simplest graph has nodes, which is the case of the original phaseonium proposal Scully et al. (2003). The interplay between quantum coherence and energy discussed in photon Carnot engine Scully et al. (2003) revealed that the energy content of the phaseonium with can be optimized at a certain phase of the coherence. We could envision as if we are considering more complex, larger, phaseonium molecules with the graphs having , corresponding to level atom phaseonium (NLAP).
We can imagine different phaseonium molecules can be possible for a given atom of unit mass and explore how the specific energy of the atom depends on the size of the phaseonium molecule characterized by . Next to the phase of coherence, becomes another control parameter which could favourably contribute to the enhancement of the specific energy of the single atom quantum fuel. For 1, the number of coherences would scale quadratically, . If the quadratic coherence scaling could be translated into the energy content of the atomic fuel, we could overcome the cavity losses for implementation and boost the performance of quantum Carnot engine for applications. From fundamental point of view, such scaling analysis could reveal profound difference of quantum fuel from a classical resource as such a scaling cannot exist without quantum coherence. Complete graphs of phaseonium molecules serve more than a simple counting of coherences. They emphasize the generality of our question we address in the present contribution. Can we beat decoherence with the scaling advantage of quantum coherent resources?
We have recently numerically examined a superradiant quantum Otto engine Hardal and Müstecaplıoğlu (2015) which exhibits a similar scaling law of work with the number of atoms; though the efficiency is independent of the temperature and the number of atoms. Our present results are fully analytical, and for a Carnot cycle which can harvest work from a single heat bath and the scaling laws with the number of coherences are both for the work and the efficiency. Furthermore, specific energy of a superradiant cluster increase linearly with the number of atoms, while here for the single atom phaseonium fuel it is quadratic. Quantum advantage in the charging power of quantum batteries with the number of qubits has been examined very recently Binder et al. (2015). Linear scaling of work with the number of qubits is reported; while due to a quantum speed up of the operation time, the charging power scales quadratically Binder et al. (2015). The preparation of phaseonium fuel and using it in PCE can be compared to charging and discharging a single qubit quantum battery with multiple quantum coherences. Phaseonium fuel or battery allows for quadratic scaling in harvested work, efficiency, and the specific energy with the number of quantum coherences. We examined the charging or preparation cost of the phaseonium battery and compared it with the harvested work by PCE. Our result verified that the second law is obeyed in our system.
Ii NLAP model and system dynamics
The operation of photonic Carnot engine is described in Fig. 2. The working fluid of the engine is the photon gas in a high quality single mode cavity of frequency . The radiation pressure by the cavity photons applies on the cavity mirrors playing the role of the piston of the engine. The quantum fuel of the engine is an NLAP. The quantum Carnot cycle consists of two quantum isothermal and two quantum adiabatic processes.
In the isothermal expansion, NLAPs are generated and injected into the cavity at a rate . The interaction time between an NLAP and the cavity field is short, , so that only one NLAP can be present in the cavity Filipowicz et al. (1986). Coherences in NLAP are characterized by phase parameters , with . Coherent superposition states in level atom system can be generated by stimulated Raman adiabatic passage Amniat-Talab et al. (2011); Bevilacqua et al. (2013), Morris-Shore transformation Saadati-Niari and Amniat-Talab (2014), or quantum Householder reflection techniques Ivanov et al. (2006, 2007). Thermalization of the single atom can be considered relatively fast and hence the injection rate would be limited by the time of coherence preparation. The choice of specific technique of coherence induction depends on the details of a particular implementation. If the amplitudes of the coherences are much smaller than the level populations, then NLAP can be assumed in an approximate thermal equilibrium with a thermal reservoir (hohlraum) at a temperature . During the interaction, the mean number of photons, , and the cavity temperature increases; while the expansion cools down the cavity when there is no atom inside. Repeated injection of NLAPs into the cavity maintains the cavity field at a temperature by transferring a total amount of heat into the cavity as . is an effective temperature defined in terms of the steady state photon number as , with is the Boltzman constant. It can be higher than in the presence of coherence Scully et al. (2003). The cavity volume, and hence the frequency, change negligibly, .
The cycle continues with an adiabatic expansion where the entropy remains constant and the temperature drops as the changes appreciably. Following step is the isothermal compression in which heat is transferred from cavity to a cold reservoir at a temperature . The cycle is completed by adiabatic compression where the temperature is raised back to .
The net work extracted from the cycle is where and . The mean photon number and the temperature at the beginning of the stage determine the entropy by . Using , , , and , we write . The efficiency of the engine is defined as . It reduces to . This coincides with the standard definition of thermodynamic efficiency in Carnot cycle and used in the original proposal of the phaseonium fuel Scully et al. (2003); Scully (2002); Rostovtsev et al. (2003); Zubairy (2002) as well as in the arguments against its feasibility in the presence of decoherence channels Quan et al. (2006). In order to present results comparable to the previous works, we calculate the efficiency as defined by these studies. To avoid any misleading impressions however, we emphasize that in practical considerations round trip efficiency can be more relevant figure of merit. The round trip efficiency of the engine should include the cost of the preparation of the quantum coherent atom; which would ensure the validity of the second law Zubairy (2002). On the other hand, it was noted that the cost of quantum fuel can be expensive Scully (2002), but it is still appealing as it can be used to harvest work from a single heat reservoir. Our objective here is not to discuss if such PCEs can be efficient enough for certain applications, but to examine if such devices, proposed in Scully et al. (2003), can produce positive work in the presence of decoherence by exploiting a scaling advantage of multiple coherence resources, in contrast to the negative conclusions of earlier studies Quan et al. (2006).
During the adiabatic process does not change so that and . These relations reveal that work and efficiency of the photonic Carnot engine can be calculated by determining the at the end of the isothermal expansion stage.
This manuscript organised as follws: In Sec. II, we describe the N-level phaseonium model, and PCE system dynamics. We review and discuss the analytical and numerical verification of the analytical results in Sec. III. We also estimate the preparation cost of NLAP in this section. We conclude the results in Sec. IV.
Iii Results and discussions
In order to find the , we solve where . Here is the Fock number state for the cavity photons and is the reduced density matrix of the cavity field. The equation of motion for can be obtained by tracing the equation of motion of the complete system over atomic degrees of freedom
where is the Hamiltonian of the arbitrary atom in the interaction picture relative to the cavity photons, with and . Here , are the energies of atomic states and , with , is the coupling rate between the atom and the field, and is the photon annihilation operator. The model Hamiltonian describes a situation where level atom is coupled to a single mode cavity in a fan shaped transition scheme. A more realistic model requires consideration of multimode cavity coupled to an atom with multiple upper and lower hyperfine levels Birnbaum et al. (2005); Arnold et al. (2011). Such models can be reduced to effective single mode cavity and multilevel atom interactions Birnbaum et al. (2005) or can be directly described by generalized master equations of micromasers Reshetov and Yevseyev (2004). Atoms with fan shaped degenerate level schemes are also studied from the perspective of generating large superposition states Kyoseva and Vitanov (2006); Amniat-Talab et al. (2011). The central question for us here is the dependence of work and efficiency on the number of the superposed quantum states and we will only consider single upper level and a set of degenerate or non-degenerate lower levels for simplicity.
Analytically calculating the right hand side of the Eq. (1), we find (see Appendix for details)
where the coefficients and depend on the atomic relaxation rate , atomic dephasing rate , detuning parameter , with , and , as well as the coherence parameters and , by the relations given in the Appendix. Thus, we obtain the rate of change of average photon number
where and .
The equation of motion for the evolution of population elements in the density matrix coincides with the thermalization dynamics of a resonator coupled to a heat bath. Accordingly, the coarse grained dynamics effectively describes sequence of NLAP injected into the resonator as a mesoscopic ensemble of level atoms acting as a heat bath. The off diagonal elements of the density matrix or the coherences can be kept vanishingly small to describe the steady state approximately as a thermal equilibrium state. The corresponding effective temperature can be determined by the modified detailed balance condition to reach such a quasi equilibrium state in Eq. (III) which gives
The detailed balance between the thermal reservoir at and the photon gas in the resonator is broken but there is a modified detailed balance between the coherent atomic ensemble and the resonator photons. Accordingly the resonator can reach a thermal equilibrium at a different temperature than .
The steady state of the Eq. (3) yields the average photon number as
where is the average photon number in the absence of coherence. Using , we determine the effective cavity temperature as
by using high temperature approximations and in Eq. (5).
Therefore, the efficiency of the photonic Carnot engine in the case of NLAP becomes
where is the Carnot efficiency. Note that for , but could have a positive value for particular values of control parameters . In order to get further analytical results we will make some simplifying assumptions.
We focus on degenerate NLAP case to proceed analytically, for which , , , , and . In addition, we consider phase locked equal amplitude coherences with and . Hence the coefficients in Eq. (III) become , and , and hence Eq. (3) reduces to
for , , where , , with . Here we introduced and , with , as the decoherence rate due to the dissipation in the cavity and a phenomenological decoherence factor due to atomic dephasing, respectively Quan et al. (2006). While the dephasing factor is phenomenologically introduced in Quan et al. (2006) we provide its rigorous microscopic derivation in the Appendix.
Steady state solution of Eq. (8) yields an effective temperature given by in the high temperature limit where
with . For small coherence and decoherence terms in , an approximate expression can be written for the effective temperature
This result shows that if the reduction of the magnitude of coherence due to dephasing is slower than the quadratic increase with , then the multilevel coherence could be used to beat the decoherence induced by the cavity dissipation. The magnitude of coherence is limited by the positivity requirement of the density matrix as well as the thermal equilibrium requirement of the cavity field. The former condition require so that for as for . Accordingly one can fix the coherence amplitude as a constant as long as it remains smaller than for the range of values. For a realistic number of levels this is not a very restrictive condition. More severe limitation on is due to the quasi-equilibrium condition of the photon gas. We will take and consider in our numerical examinations. In the classical asymptotical limit of then as and hence the quadratic scaling reduces to a linear one for which the specific energy becomes a constant as expected for classical systems. Mesoscopic systems in quantum regime are therefore necessary to exploit the quadratic scaling in the specific energy.
We note that the coarse grained dynamics is designed on purpose to determine the steady state by rapid convergence using a numerically efficient dynamical equations. Analytical solution of the mean photon number dynamics for the degenerate case and with , , gives
where is the thermalization time. We will first discuss the predicted analytical state states by the coarse grained master equation in modern resonator settings then examine the exact numerical desription of the dynamics of the system to verify the analytical results in the subsequent subsections.
iii.1 Analytical results for
modern resonator systems
In the high temperature limit (, the entropy change in the isothermal expansion stage is and the heat input becomes . The work output at is found to be where , respectively. In superconducting circuit, microwave and optical resonators, it is estimated that Quan et al. (2006). should be replaced by for smaller number of levels. Accordingly, by using five or more level quantum phaseonium fuel, the working fluid can beat quantum decoherence to harvest positive work.
In Fig. 3, we plot the work output and efficiency of the photonic Carnot engine with degenerate NLAP fuel, depending on the number of quantum coherent levels. We consider independent as well as dependent scaling models Yavuz (2014) for the decoherence factor and take in Fig. 3(a)-(b), in Fig. 3(c)-(d), and in Fig. 3(e)-(f), where as shown in the Appendix. The plots are given for the circuit QED parameters in Quan et al. (2006). We consider larger atomic dephasing rates than the typical values to demonstrate its limiting effect on and . The plots indicate that even when there is large dephasing, which can increase with linearly or quadratically, and can retain their quadratic power law with up to a critical .
Similar results are found for the cases of optical and microwave cavities. We see both in Fig. 4(a)-(b) and Fig. 5(a)-(b) that when dephasing is independent of , the work output and efficiency increases quadratically with the number of coherent levels. If the dephasing rate is increasing linearly with as in Fig. 4(c)-(d) and Fig. 5(c)-(d), or if it is increasing quadratically with as in Fig. 4(e)-(f) and Fig. 5(e)-(f), the work output and efficiency of the photonic engine is enhanced quadratically with the number of coherent levels only up to critical . beyond which the work output and efficiency decays exponentially due to the dominating effect of decoherence.
iii.2 Numerical verification of the theory
In order to perform a faithful numerical simulation of a typical set up described in the theory, we investigate the injection process in detail. We assume a regular atomic injection of Rydberg atoms into a Fabry-Perot cavity Raimond et al. (2001) with an atomic interaction time with the cavity field and an empty cavity time such that where is the injection rate. During the time interval , the hamiltonian is
while for the time interval , ( and for degenerate ground state levels).
We choose injection time where is the cavity decay rate and is the number of atoms kicking the cavity field in the photon lifetime. The time elapsed when cavity is empty can be related to the interaction time such that . Thus, we can write . Here, is a factor introduced to measure in terms of so that .
We solve the master equation by numerical methods and compare the results with the developed theory. We use QuTip package Johansson et al. (2012) in Python software to solve the master equation. We perform single atomic injection in two steps. First step is the atom-cavity field interaction (during ) and the second one is the free cavity field evolution (during ). The master equation for the first step is written under Markov and Born-Markov approximations as Gardiner and Zoller (2010)
where last two terms stand for pure spontaneous emission and pure dephasing Nunnenkamp et al. (2011); Jirari and Pötz (2005); Schirmer and Solomon (2004); Li et al. (2012), respectively. Here, is a Liouvillian superoperator in Lindblad form and , . We include an auxiliary state to the atomic state space to model the decay of the excited and the lower levels. Presence of is not altering the initial phaseonium state. The auxiliary state is unpopulated and at the lower level energy. Its use allows for faithful simulation of the excited state and the degenerate ground state ) decay equations in Eq. (LABEL:Eq15). This decay model is already used in the original master equation developed for the two-level phaseonium engine Rostovtsev et al. (2003). Different decay models, for example decay of excited level to the lower levels are employed for other systems such as many atom superradiant Otto engine Hardal and Müstecaplıoğlu (2015) and similar effect of beating decoherence with scaling up coherence is found. Present contribution discusses the original photo-Carnot engine Scully et al. (2003) as well as the objection to its feasibility due to dephasing, phenomenologically described by factor Quan et al. (2006). Our introduction of is an additional decoherence channel not included in Ref. Quan et al. (2006). We have found that can be analytically expressed in terms of (see Appendix for details). The microscopical master equation approach describes both the original photo-Carnot engine coarse-grained master equations with Quan et al. (2006) and without Rostovtsev et al. (2003) dephasing and generalizes them to the multilevel case; as our mesoscopic master equation, Eq. III, does analytically.
In the second step, cavity decay is present during the time interval in accordance with the key assumptions of micromaser theory Filipowicz et al. (1986) and the corresponding master equation is
In Fig. 6, we present the thermalisation process of the cavity field depending on different values by depicting the photon number versus scaled time. Physical parameters Quan et al. (2006) are given in the figure caption consistent with the Rydberg atoms in a superconducting Febry-Perot cavity Raimond et al. (2001). For low values of which corresponds to large , we have zigzag like curves and for high values of , we have smoother lines. Average photon number converges to the theoretical value for . Thermalisation time is much longer than the convergence rate of coarse grained master equation and the microscopic exact method is much more costly numerically.
In Fig. 7(a)-(b), we express the effect of the number of degenerate atomic ground state levels of the coherent atoms against the dephasing and the cavity loss mechanisms. Horizontal dotted and dotted-dashed lines are the analitical values of average photon numbers ( , ) of the no loss case for each . In Fig. 7(a) when decoherence channels are open, average photon number saturates below the analytical values for in accordance with the argument that 2LAP phaseonium can not beat decoherence Quan et al. (2006). Average photon number exceeds for in Fig. 7(b) by keeping all the other parameters same. Thus, we show that the decoherence can be beaten by using higher . To make the effect more visible in the figures, we take larger coherence magnitude, .
We also compare the consistency of effective field temperature T, harvested work and efficiency versus in Fig. 8 (a), (b), (c) between developed analytical and numerical results when dissipation channels open. We observe a good consistency between numerical and theoretical results in steady state.
iii.3 Preparation of the NLAP
and its energy cost
Typical methods to generate quantum superposition states, such as pulse area, adiabatic passage, or STIRAP techniques Amniat-Talab et al. (2011); Bevilacqua et al. (2013), utilize optical pulses interacting with the atomic system to transfer an initial atomic state to a target one. The initial and target quantum states are known and hence one can easily determine the required unitary transformation between them. Physical implementation of the required propagator is however a much more challenging problem than the calculation of the transformation matrix. An efficient strategy to sythesize the transformation matrix is to decompose it into a product of matrices, representing interacting steps that can be implemented by using optical pulses coupled to the atom.
An arbitrary dimensional unitary matrix can be decomposed into so called generalized quantum Householder reflection (QHR) matrices or standard QHRs and a phase gate Ivanov et al. (2006, 2007). A generalized QHR is defined by
where is the identity operator and the is the normalized column vector with dimension , same with the number of the pulses, and is an arbitrary phase factor. The decomposition of in terms of generalized QHRs can be written as
For , Eq. (15) reduces to which is the standard QHR. The interaction represented by each Householder matrix can be described by a propagator which can be determined by the Morris-Shore transformation Saadati-Niari and Amniat-Talab (2014).
Our N+1 level atom coupled to N optical pulses in a fan shaped transition scheme, or so called N-pod model, is a generic model that is used to discuss generation of arbitrary multilevel superposition states. Under the Morris-Shore transformation, the lower levels of the atom are grouped into a single bright level coupled to an effective single pulse and N-1 dark levels uncoupled from the optical pulses. The propagator is then easily determined in this Morris-Shore basis. Back transformation to the original basis gives the full propagator, or the generalized QHR matrix. Both the number of QHR steps and the number of pulses used in each step are in the order of , therefore the total number of pulses to be used to generate the target state would be in the order of . This shows that the energetic cost of preparation of the target state scales with , same with the work and efficiency scaling in the corresponding photonic Carnot engine.
The preceding discussion is applicable to the case of mixed states as well, for which the normalized vectors of generalized QHRs are defined as Ivanov et al. (2006)
Here, is the column of , and is an arbitrary phase where . It’s shown that for an N-Pod system any standard QHR can be realized by single pulses with an rms pulse area Ivanov et al. (2007). The corresponding unitary transformation can only link the mixed states with the identical dynamical invariants. In our case we consider initial thermal states out of a hohlarum transformed to a final state with small coherences. The initial and final states would then possess different spectral decompositions so that they cannot be unitarily connected. A resolution to this is suggested to exploit decoherence channels such as spontaneous emission or pure dephasing, in combination with the unitary transformation Ivanov et al. (2006, 2007). We will not follow this route but use an alternative, which allows for a fully unitary procedure to generate desired coherences. As the coherences contribute additively, to exploit their scaling advantage we do not need an exact state but an approximate one would be sufficient. Accordingly, we can simply consider an approximate approach and do not specify an exact value for the coherences. We only need to keep them small enough to ensure slightly out of thermal equilibrium final state. We illustrate our strategy for case, and suggest that in principle larger NLAP can be generated by straightforward extension of this technique. Unitarity of our procedure also makes the details of generation process immaterial for the cost estimation. The cost would be the same for other unitary equivalent processes to generate same states.
Initial state of the atom out of the hohlarum at is the thermal density matrix
where inverse temperature and is the partition function, with being the atomic Hamiltonian. Taking and , we find . Target density matrix is taken to be
where the off-diagonal elements between degenerate ground state levels are taken real and much smaller than the diagonal elements that are equal to those of the . The initial and final density matrices have distinct dynamical invariants in their spectral decompositions and hence they cannot be linked by a coherent evolution. Let us assume however an approximate link such that . The unitary transformation can be determined from the matrix that diagonalize and found to be
Writing , the fidelity between and is determined by and found be . Thus, can be approximately be used as the unitary operator linking the initial and the target density matrices.
can be synthesized by using two standard QHRs and a phase gate as
where and is a one-dimensional phase gate. By using Eq. (17) one finds the normalized column vectors to be , . The example for here illustrates the basic principles to generate arbitrary NLAP. One can use pulses for each standard QHRs and a phase gate to synthesize a unitary transformation matrix, which is the diagonalization matrix of a quasi equilibrium thermal state at with small coherences. When the pulses applied to the actual atom out of hohlarum at , the final state will be approximately the same with the target state used to determine the properties of the pulses.
We can now estimate the energy cost of generating using where is the total number of pulses used in the QHR technique and is the energy of a single pulse. can be determined from the pulse area as in Hardal and Müstecaplıoğlu (2015). For a square pulse of duration and amplitude we have , where is the magnitude of the dipole moment
where is the vacuum permittivity and is the speed of light. Taking the pulse area we find
The intensity of the pulse is given by . The pulse energy in a beam of radius can be estimated by . Using and , where and are the wavelength of the optical field and the radial beam divergence, respectively, we find
Taking and Hardal and Müstecaplıoğlu (2015), we find .
Total energy cost to reach steady state per cycle is where . Here, is the number of atoms needed for thermalisation, is the injection rate, and is the time elapsed to reach the steady state. In our results we have found that the harvested work per cycle is much less than the resonance energy, , thus the generation cost of NLAP fuel is several orders of magnitude larger than the harvested work , which confirms that the second law of thermodynamics obeyed in photonic Carnot engine with NLAP. Generation cost is not included in the thermodynamic efficiency but it can be significant figure of merit in the round trip efficiency. To make such photonic Carnot engines more appealing for certain applications, it is necessary to increase their round trip efficiency as well. For that aim one could consider the cases of larger compression ratios () and high operation temperatures (). Our focus here is on the discussion if such engines can operate under decoherence. Despite the negative conclusions for two level phaseonium case Quan et al. (2006), we have found that larger phaseonium fuel allows for operational photonic Carnot engines. The question of how to increase their round trip efficiency requires further analysis which is beyond the scope of present contribution.
Summarizing, we examined scaling of work and efficiency of a quantum heat engine with the number of quantum resources. Specifically, we considered a photonic Carnot engine with a multilevel phaseonium quantum fuel. We derived a generalized master equation for the cavity photons, which forms the working fluid of the engine, and determined the steady state photon number to calculate the work output and thermodynamic efficiency. We find that they scale quadratically with the number of quantum coherent levels . We examined the case of degenerate levels to get analytical results and to examine scaling laws against decoherence due to cavity dissipation and atomic dephasing. We verified our analytical results with detailed numerical methods and have shown consistency of coarse grained analytical results with the microscopical numerical approach. Generation of multilevel phaseonium fuel using Morris-Shore transformation determined quantum HousehoÄ±lder reflection technique as well as its cost are examined. Using typical parameters in modern resonator systems, such as circuit QED, our calculations reveal that decoherence due to cavity dissipation could be overcome by the multilevel quantum coherence even in the presence of large dephasing rate. If the dephasing rate increases with , then work and efficiency can still overcome the decoherence and retain their scaling up to a critical number of coherent levels.
Authors warmly thank N. Allen, A. Imamoglu and I. Adagideli for illuminating discussions. Authors acknowledge support from Koç University and Lockheed Martin University Research Agreement.
We generalize micromaser mesoscopic master equation treatment Rostovtsev et al. (2003) applied for three-level phaseonium engine Scully et al. (2003) to multi-level case. In LAP model, the Hamiltonian of the whole system is where label implies injected arbitrary atom. We adopt the notation of ref. Lu and Bergou (1989) for the Hamiltonian and relevant quantities. Here, and
in the interaction picture where , are atomic energy levels, is the atom-field coupling coefficient and is the single mode cavity frequency. Here, we assume all levels coupled to the excited one with the same coefficient . The equation of motion of overall system is
where and are the Liouvillian superoperators expressed in the main text corresponding to atomic and field degrees of freedom respectively.
The equation of motion of the radiation field which is the working substance of the heat engine can be found by tracing out atomic part as
where . Here, . In micromaser theory, due to the short atom-cavity interaction time, last term, cavity decay is usually ignored when the atom is inside the cavity. The second term is treated perturbatively and will be considered for zeroth order in g. Here, we will keep it but assume it can be treated independently. One may write the partial trace operation over atomic degrees of freedom for a random single atom as,
where are the atomic basis as expressed at the right hand side. Each term of Eq. (28) can be calculated by using the selective rules of the Hamiltonian between certain levels and ; for instance inserting for the first term of Eq. (28) we have,
where and . Expressing the terms of Eq. (29) conveniently, we write
Inserting these results into Eq. (27) and after some rearrangements we have the field equation of motion,
We use hereafter for simplicity. Here,
In order to proceed the calculation, any single term in the summation of Eq. (34) should be calculated and inserted therein. The terms can be obtained by the integration of corresponding equation of motions by using the selecetive rules of the Hamiltonian as expressed above. We evaluate atomic equation of motion order in first, we have
where and . Final two terms of Eq. (36) corresponds to with and