Abstract
Feedback control mechanisms are ubiquitous in science and technology, and play an essential role in regulating physical, biological and engineering systems. The standard second law of thermodynamics does not hold in the presence of measurement and feedback. Most studies so far have extended the second law for discrete, Markovian feedback protocols; however, nonMarkovian feedback is omnipresent in processes where the control signal is applied with a nonnegligible delay. Here, we experimentally investigate the thermodynamics of continuous, timedelayed feedback control using the motion of an optically levitated, underdamped microparticle. We test the validity of a generalized second law which bounds the energy extracted from the system, and study the breakdown of feedback cooling for very large time delays.
Introduction
The second law of thermodynamics is of fundamental and practical importance^{1}. On the one hand, it allows one to predict which transformations are possible in nature. On the other hand, it offers a method for determining the efficiency of a given process by comparing it to its ideal, reversible limit. According to the standard formulation of the second law, no work can be cyclically extracted from a system coupled to a single reservoir at temperature T_{0}, that is, the power output has to be negative, \({\dot{{\mathcal{W}}}}_{\text{ext}}\ \le \ 0\)^{1}. However, in the presence of measurement and feedback, this statement of the second law breaks down and positive work can be produced, as exemplified by Maxwell’s and Szilard’s thought experiments^{2,3}. For Markovian feedback protocols a refined version of the second law reads \({\dot{{\mathcal{W}}}}_{\text{ext}}\ \le \ {k}_{\text{B}}{T}_{0}{\dot{{\mathcal{I}}}}_{\,\text{flow}}^{\text{mar}\,}\), where T_{0} is the bath temperature and \({\dot{{\mathcal{I}}}}_{\,\text{flow}}^{\text{mar}\,}\) is the information flow to the detector, defined as the time variation of the mutual information between a variable and its measured value^{4,5,6}. This inequality has been experimentally verified with colloidal particles^{7,8} and single electrons^{9,10}. When the information rate \({\dot{{\mathcal{I}}}}_{\,\text{flow}}^{\text{mar}\,}\) is positive, more work can be extracted from the system than permitted by the usual second law of thermodynamics.
The fact that a control signal cannot be applied instantaneously implies that feedback circuits inevitably exhibit memory effects and are thus nonMarkovian. The Markovian approximation is only valid when the delay, i.e., the time between measurement and feedback, is much smaller than the typical timescales of the system. Delayed feedback is widespread in many areas, from chaotic systems to biology^{11,12,13,14,15}, emphasizing the crucial need to expand the second law to account for finite memory. However, such generalization is nontrivial. Because of the nonMarkovian nature of the feedback, the conventional approach of stochastic thermodynamics^{16} cannot be applied and the usual condition of local detailed balance does not hold. As a result, new contributions to the nonequilibrium entropy production occur, leading to the extended second law for continuous, nonMarkovian feedback, \({\dot{{\mathcal{W}}}}_{\text{ext}}\ \le \ {k}_{\text{B}}{T}_{0}{\dot{{\mathcal{S}}}}_{\text{pump}}\), where \({\dot{{\mathcal{S}}}}_{\text{pump}}\) is the entropy pumping rate, which incorporates the effect of the time delay^{17,18,19,20}. Since \({\dot{{\mathcal{S}}}}_{\text{pump}}\ \le \ {\dot{{\mathcal{I}}}}_{\,\text{flow}}^{\text{mar}\,}\), this is the tightest secondlaw inequality to date^{18}. Despite the omnipresence of delay in feedback processes, a dedicated experimental investigation of this nonMarkovian generalization of the secondlaw inequality is still lacking.
Here, we report the experimental study of the thermodynamics of continuous, nonMarkovian feedback control applied to the underdamped centerofmass (CM) motion of a levitated microsphere^{21}. Levitated particles are an ideal experimental platform to explore thermodynamics in small systems^{22,23,24,25,26,27}. We confirm the validity of the generalized second law for time delays spanning two decades and observe the breakdown of the highqualityfactor (high Q) approximation^{18}. We establish that the efficiency of the feedback is enhanced when nonMarkovian effects are included. We further explore the relation between Markovian and nonMarkovian feedback by analyzing how the delay affects the correlations between measurement outcome and velocity of the particle. We finally explore the limitations of feedback cooling and the saturation of the effective CM temperature of the system above the bath temperature for very large delay.
Results
Generalized second law
We consider a harmonic oscillator in contact with a heat bath at temperature T_{0}, and subjected to a delayed feedback control that acts as an information reservoir (Fig. 1). Delayed feedback control means here that we acquire information about the oscillator position x_{t} at time t and apply a force \({F}_{\text{fb}}(t)\propto {x}_{t{t}_{\text{fb}}}\) to manipulate its motion based on the position measured at time t − t_{fb}. The stochastic dynamics of the oscillator is governed by the underdamped Langevin equation^{28},
with m the particle mass, Ω_{0} its natural frequency, and Γ_{0} the damping coefficient. The quantity ξ_{t} is a centered Gaussian white noise with \(\langle \xi (t)\xi (t^{\prime} )\rangle =\delta (tt^{\prime} )\). The linear feedback is applied via the force \({F}_{\text{fb}}=gm{\Gamma }_{0}{\Omega }_{0}{x}_{t{t}_{\text{fb}}}\) with feedback gain g > 0^{18}. The mechanical quality factor of the resonator is given by Q_{0} = Ω_{0}∕Γ_{0} and the feedback damping rate by Γ_{fb} = gΓ_{0}. It is convenient to introduce the normalized delay τ = t_{fb}Ω_{0} and the position of the oscillator normalized to its standard deviation in equilibrium^{17,18,19,20}. The dynamics of the particle is then fully characterized by a set of dimensionless parameters (g, Q_{0}, τ) (Methods). Both the harmonic and Brownian terms in Eq. (1) are Markovian. Memory effects enter only via the delayed feedback force F_{fb}.
When the feedback force acts to cool the harmonic oscillator, the extracted work \({{\mathcal{W}}}_{\text{ext}}={\mathcal{W}}\) is taken to be positive. According to the first law, the energy balance reads \(\Delta U={\mathcal{W}}{\mathcal{Q}}\). As a result, the heat dissipated into the heat bath in the steady state is \({\mathcal{Q}}={{\mathcal{W}}}_{\text{ext}}\). On the other hand, the steadystate entropy balance is^{17,18,19,20}
where \({\dot{{\mathcal{S}}}}_{\text{pump}}\) is the entropy pumping rate, an additional contribution to the entropy production that stems from the feedback control and depends on the delay for nonMarkovian protocols. The entropy pumping rate is computed by coarsegraining the harmonic and feedback forces over the position variable^{17,18,19,20} (Methods). For a harmonic potential and a linear feedback force, the velocity distribution is a Gaussian (Fig. 2b), \(P(v)=\exp \left({v}^{2}/2{\sigma }_{v}^{2}\right)/\sqrt{2\pi {\sigma }_{v}^{2}}\) with variance \({\sigma }_{v}^{2}\). The nonMarkovian feedback control leads to a cooling of the microparticle, corresponding to negative entropy pumping and extracted work rates, when \({\sigma }_{v}^{2}\,{<}\,1\). By contrast, heating occurs for \({\sigma }_{v}^{2}\,{> }\, 1\).
The validity of inequality (2) can be assessed by comparing the entropy pumping to Markovian bounds. The usual Markovian velocity feedback (VFB) cooling^{29,30}, with a feedback force proportional to the instantaneous velocity of the particle, F_{fb} ∝ − v, is recovered in the limit of Q_{0} ≫ τ and for τ = π∕2 + 2πn, with n an integer. The entropy pumping rate corresponds in this case to \({\dot{{\mathcal{S}}}}_{\text{vfb}}=g/{Q}_{0}\)^{31}, which we identify as the Markovian information flow \({\dot{{\mathcal{I}}}}_{\,\text{flow}}^{\text{mar}\,}\) (Methods). The highqualityfactor approximation (Q_{0} ≫ 1) allows one to map the nonMarkovian dynamics to an effectively Markovian Langevin equation, because the motion of the oscillator is essentially coherent on that timescale^{18}. The effect of the feedback is then incorporated in a modified damping \(\Gamma ^{\prime} ={\Gamma }_{0}(1+g\sin \tau )\) and mechanical frequency \(\Omega {^{\prime} }^{2}={\Omega }_{0}^{2}[1({\Gamma }_{\text{fb}}/{\Omega }_{0})\cos \tau ]\) of the resonator (Supplementary Note 2). The Markovian second law remains valid with these modified parameters. In the high Q approximation, the entropy pumping is given by \({\dot{{\mathcal{S}}}}_{\text{highQ}}=(g/{Q}_{0})\sin \tau\)^{18}. The approximation is expected to breakdown for larger τ, when the Brownian force noise leads to dephasing between the oscillator motion and the feedback signal. This regime can only be correctly described using the generalized second law (2).
Experimental setup and results
In our experiment, we use an optically levitated microparticle to implement the dynamics of Eq. (1), which holds for any harmonic system with linear feedback control. A standing wave is formed by two counterpropagating laser beams (λ = 1064 nm) inside a hollowcore photonic crystal fiber (HCPCF) (Fig. 2a and Methods)^{21}. A silica microsphere (969nm diameter) is trapped at an intensity maximum of the standing wave. The amplitude of the particle motion is sufficiently small to allow for a harmonic approximation of the potential with frequency Ω_{0}∕2π = 404 kHz (Supplementary Note 7). The damping coefficient Γ_{0} as well as the bath temperature T_{0} = 293 K are determined by the surrounding gas. In our setup, the linear dependence of the damping coefficient Γ_{0} on the environmental pressure allows simple and systematic tuning of this parameter along with the mechanical quality factor Q_{0} = Ω_{0} ∕ Γ_{0}. The particle motion along the xaxis is detected by interferometric readout of the light scattered by the particle^{21}. The signal is fed into a delay line that is digitally implemented, and the output signal serves to control the power of a feedback laser. This laser exerts a radiation pressure force in one direction, accelerating the microparticle proportional to the delayed particle position. The overall amplification of the signal sets the proportionality constant, which is given by gΩ_{0}Γ_{0}, where the gain in our experiment is g = 0.36 (Supplementary Note 5). The whole feedback circuit has a minimal delay of t_{fb} = 2.6 μs, i.e., τ = 2.04π.
We first test the extended second law (2) by varying the delay over two decades. Figure 3a demonstrates the validity of the nonMarkovian inequality (2) over all relevant timescales. The nonMarkovian entropy pumping rate \({\dot{{\mathcal{S}}}}_{\text{pump}}\) (green) is a much more precise upper bound to the extracted work rate (black) than the Markovian pumping rate \({\dot{{\mathcal{S}}}}_{\text{vfb}}\) (horizontal dashed line). In particular, the Markovian result fails to capture the oscillations of the extracted work rate, as well as the heating phases induced by the delay. The high Q approximation (dasheddotted line) correctly describes the oscillatory behavior of \({\dot{{\mathcal{S}}}}_{\text{pump}}\) for short delays. Yet, it does not account for the oscillation decrease induced by the Brownian force noise for long delays. We already observe significant deviations for a delay of only three oscillation periods with a mechanical quality factor of Q_{0} = 55. We have also verified the second law (2) by varying the dissipation via Q_{0} (Supplementary Note 9).
The generalized second law (2) is crucial to properly estimate the performance of the feedback cooling. In analogy to heat engines and refrigerators, one may define the efficiency of work extraction \({\eta }_{\text{pump}}={\dot{{\mathcal{W}}}}_{\text{ext}}/({k}_{B}{T}_{0}{\dot{{\mathcal{S}}}}_{\text{pump}})\), which characterizes the conversion of information into extracted work^{32}. As shown in Fig. 3b, the corresponding Markovian efficiencies for velocity feedback (η_{vfb}) and for the high Q approximation (η_{highQ}) vastly underestimate the feedback efficiency. We note that the pumping efficiency η_{pump} and cooling power \({\dot{{\mathcal{W}}}}_{\text{ext}}\) exhibit a tradeoff similar to that of heat engines: one is maximal when the other is minimal, and vice versa. By contrast, the velocity feedback efficiency η_{vfb} exhibits an opposite dependence on τ.
We may gain physical insight on the breakdown of the standard second law as shown in Fig. 3 by analyzing the correlations between particle velocity and feedback force, as well as the effective temperature of the system. Cooling is efficient when the feedback force counteracts the motion of the oscillator, in other words, when the velocity v_{t} of the oscillator and the feedback force (F ∝ x_{t−τ}) are anticorrelated. Heating occurs when they are correlated. Figure 4 shows the correlation function between the two quantities, c(τ) = 1∕(σ_{q}σ_{v})∫∫y_{t}v_{t}P(y_{t}, v_{t})dy_{t}dv_{t} with y_{t} = q_{t−τ} (Supplementary Note 4). The delay τ has two effects. First, it changes the phase between the mechanical system and the feedback signal deterministically, resulting in the oscillatory behavior of the correlations, and thus the difference between heating and cooling. Second, it allows for stochastic dephasing of the mechanical motion with respect to the feedback signal, which translates into a reduction of the correlations for increasing delay. These correlations do not vanish, however, but asymptotically approach a finite value. For long delays, the oscillator thermalizes due to the damping. The action of the feedback circuit can then be seen as an independent force noise with the spectrum of a whitenoise driven harmonic oscillator. The positive correlations occur as a result of the resonant driving of the mechanical motion by the feedback signal.
Figure 5 displays the ratio of the effective steadystate temperature, \({T}_{\text{eff}}={T}_{0}{\sigma }_{q}^{2}\)^{18}, and the bath temperature T_{0}. Figure 5a clearly shows how the action of the feedback is reduced when the mechanical quality factor Q_{0} is decreased or the time delay τ increased. For all values of Q_{0}, there is a certain delay τ, beyond which cooling is no longer possible (black line). For even longer delays, the effective temperature reaches a constant value, \({T}_{\,\text{eff}\,}^{\infty }/{T}_{0}\approx 1+{g}^{2}/2\), that is independent of Q_{0} for weak coupling g ≪ Q_{0} (Supplementary Note 3). This is in line with the second law that predicts an asymptotic negative work extraction, \({{\mathcal{W}}}_{\,\text{ext}\,}^{\infty }\approx {g}^{2}/(2{Q}_{0})\) for very long delays. Figure 5b provides a cut for constant Q_{0} = 55 through Fig. 5a. The grayshaded area on the right shows the region where T_{eff} > T_{0} for our gain g = 0.36. Note that this region can be reduced by decreasing the feedback gain. Excellent agreement between theory (red) and data (black) is observed.
Discussion
In summary, we have performed an extensive experimental study of the second law of thermodynamics in the presence of continuous nonMarkovian feedback. Our results constitute an important step toward bridging theoretical developments in stochastic information thermodynamics and more technical applications like continuous feedback. Possible generalizations include the consideration of measurement noise^{31} and the extension to nonlinear potentials and nonlinear feedback (e.g., parametric cooling of levitated nanoparticles^{33}). Nonlinear delayed feedback control has thus already proven to be a more robust and effective method for synchronization compared with its linear counterpart^{34}. Another avenue of future research is the use of optimal control via Kalman–Bucy filters^{20}. Intuitively, one might hope that elaborate filtering methods, like Kalman filters, may overcome the impact of delay that we observe in our simple feedback scenario by an optimal prediction of the instantaneous velocity. However, while this will help to reduce the effect of measurement noise, the effect of stochastic Brownian force noise that occurs during the delay is fundamentally unpredictable. We therefore anticipate no improvement compared with the longdelay results presented in our work.
Methods
Normalized form of the equation of motion
After time contraction t → tΩ_{0} and position normalization x → q = x∕x_{th} with \({x}_{\text{th}}=\sqrt{{k}_{\text{B}}{T}_{0}/m{\Omega }^{2}}\) the thermal root mean square amplitude, the Langevin equation can be rewritten in the dimensionless form,
with Q_{0} = Ω_{0}∕Γ_{0} the quality factor, g = Γ_{fb}∕Γ_{0} the feedback gain, τ = t_{fb}Ω_{0} the normalized delay and ξ_{t} representing a centered Gaussian white noise force with \(\langle \xi (t)\xi (t^{\prime} )\rangle =\delta (tt^{\prime} )\).
Experimental setup
The particle is trapped in an intensity maximum of the standing wave and oscillates in a harmonic trap. For a laser power of 400 mW in each trapping beam, the mechanical frequency is Ω_{0}∕2π = 404 kHz. The particle CM motion is recorded using a balanced photodiode and roughly 10% of the light transmitted through the HCPCF and that scattered by the particle. The feedback control is implemented via radiation pressure of a second laser beam which is orthogonally polarized and frequency shifted with respect to the trapping laser to avoid interference effects. The feedback force F_{fb} is realized in the following steps. The readout signal of the CM motion is bandpass filtered (bandwith: 600 kHz, center frequency: Ω_{0}∕2π) to get rid of technical noise in the detector signal. Then, the signal can be amplified and delayed by an arbitrary time t_{fb} with a field programmable gate array. This signal is then used as modulation input for the AOM. A more detailed description of the experimental setup and the feedback control can be found in Supplementary Note 6 and in ref. ^{21}
Thermodynamic quantities
The nonMarkovian entropy pumping rate \({\dot{{\mathcal{S}}}}_{\text{pump}}\) can be computed by coarsegraining the harmonic (h) and feedback (fb) forces over the position variable: \({\dot{{\mathcal{S}}}}_{\text{pump}}=\int \text{d}\,v\left[\overline{{F}_{\text{fb}}(v)}+\overline{{F}_{\text{h}}(v)}\right]{\partial }_{v}P(v)\), where P(v) is the velocity distribution and \(\overline{{F}_{\text{i}}(v)}=\int dx\overline{{F}_{\text{i}}(x,v)}P(x v)\) is the corresponding coarsegrained forces^{17,18,19,20}. On the other hand, the Markovian information flow \({\dot{{\mathcal{I}}}}_{\,\text{flow}}^{\text{mar}\,}\) in the case of VFB is given by the time variation of the mutual information between the velocity v and the measured value of the velocity y: \({\dot{{\mathcal{I}}}}_{\,\text{flow}}^{\text{mar}}=\int \text{d}v\text{d}\,y{\partial }_{v}J(v)\,\text{ln}\,[P(v,y)/P(v)P(y)]\) with the velocity probability current J(v)^{18,19,20}. This quantity diverges for errorfree feedback^{31}. We thus identify the Markovian entropy bound with the Markovian limit of \({\dot{{\mathcal{S}}}}_{\text{pump}}\to {\dot{{\mathcal{S}}}}_{\text{vfb}}=g/{Q}_{0}\)^{18,19,20}. For a harmonic potential and a linear feedback force, the velocity distribution is a Gaussian, \(P(v)=\exp \left({v}^{2}/2{\sigma }_{v}^{2}\right)/\sqrt{2\pi {\sigma }_{v}^{2}}\), with variance \({\sigma }_{v}^{2}\). The entropy pumping rate is then explicitly \({\dot{{\mathcal{S}}}}_{\text{pump}}=(1{\sigma }_{v}^{2})/({Q}_{0}{\sigma }_{v}^{2})\) and the work extraction rate reads \({\dot{{\mathcal{W}}}}_{\text{ext}}/({k}_{\mathrm{B}}{T}_{0})=(1{\sigma }_{v}^{2})/{Q}_{0}\) (Supplementary Note 1). We experimentally obtain the velocity variance needed to verify the generalized second law as follows: for a given time delay τ, a position time trace x(t) is recorded, filtered with a bandwidth of 3Γ_{0} via post processing, and normalized with the standard deviation of the feedback beam turned off, to find the normalized position q(t). The velocity \(v=\dot{q}\) is then numerically calculated with the finite difference approximation and the variance \({\sigma }_{v}^{2}\) computed.
Data availability
The datasets generated in the current study are available from MD on reasonable request.
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Acknowledgements
We thank Markus Aspelmeyer for valuable discussions and support, and James Millen for helpful comments. N.K. acknowledges support from the Austrian Science Fund (FWF): Y 952N36, START. D.G. acknowledges support through the doctoral school CoQuS (Project W1210). We further acknowledge financial support from the German Science Foundation (DFG) under project FOR 2724.
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M.D. and D.G. carried out experiments and analyzed data. N.K. and E.L conceived the experiment. J.J.A. and E.L. supported theoretical aspects. All authors discussed the results and contributed to the interpretation of the data and writing of the paper.
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Debiossac, M., Grass, D., Alonso, J.J. et al. Thermodynamics of continuous nonMarkovian feedback control. Nat Commun 11, 1360 (2020). https://doi.org/10.1038/s41467020151485
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DOI: https://doi.org/10.1038/s41467020151485
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