Quantum many-body scars or Non-ergodic Quantum Dynamics in Highly Excited States of a Kinematically Constrained Rydberg Chain Christopher J. Turner1, A. A. Michailidis1, D. A. Abanin2, M. Serbyn3, Z. Papi´c1 1School of Physics and Astronomy, University of Leeds 2Department of Theoretical Physics, University of Geneva 3IST Austria 15th December 2017 Lancaster, NQM2 arXiv:1711.03528 Outline What is a quantum scar? 1.0 L = 28 An experimental phenomena L = 32 0.8 2 i | ) t ( 0.6 2 Z | 2 0.4 4 Z Exact L Why is it happening? | h 2 0.2 FSA i | ψ 2 0.0 | n 0 10 20 30 t | h 0 What else is going on? 2 L 2 i | ψ 1 | n | h 0 0 10 20 30 n Quantum scars I First discussed by Heller 1984 in quantum stadium billiards. I Here, classically unstable periodic orbits of the stadium billiards (right) scarring a wavefunction (left). I One might expect unstable classical period orbits to be lost in the transition to quantum mechanics as the particle becomes \blurred". I This model is quantum ergodic but not quantum unique ergodic1. Think eigenstate thermalisation for all eigenstates vs. almost all eigenstates. 1Hassell 2010. ARTICLE doi:10.1038/nature24622 Probing many-body dynamics on a 51-atom quantum simulator Hannes Bernien1, Sylvain Schwartz1,2, Alexander Keesling1, Harry Levine1, Ahmed Omran1, Hannes Pichler1,3, Soonwon Choi1, Alexander S. Zibrov1, Manuel Endres4, Markus Greiner1, Vladan Vuletić2 & Mikhail D. Lukin1 Controllable, coherent many-body systems can provide insights into the fundamental properties of quantum matter, enable the realization of new quantum phases and could ultimately lead to computational systems that outperform existing computers based2 on classical approaches. Here we demonstrate a method for creating controlled many-body This experimentquantum matter that combinesreports deterministically on a prepared, Rydberg reconfigurable chain arrays of individually with individual trapped cold atoms with strong, coherent interactions enabled by excitation to Rydberg states. We realize a programmable Ising-type quantum controlspin over model with interactions. tunable interactions and systemThe sizes Hamiltonian of up to 51 qubits. Within isthis model, we observe phase transitions into spatially ordered states that break various discrete symmetries, verify the high-fidelity preparation of these states and investigate the dynamics across the phase transition in large arrays of atoms. In particular, we observe robust many- body dynamics correspondingX to persistentΩj oscillations of the order after aX rapid quantum quench that results from a sudden transitionH across= the phase boundary.X Ourj method∆ jprovidesnj a+ way of exploringVij many-bodyni nj phenomena on a (1) programmable quantum simulator and could2 enable− realizations of new quantum algorithms. j i<j The realization of fully controlled, coherent many-body quantum probabilistically loaded dipole trap arrays24. Our approach combines systems is an outstanding challenge in science and engineering. As these strong, controllable interactions with atom-by-atom assembly of quantum simulators, they can provide insights into strongly correlated arrays of cold neutral 87Rb atoms25–27. The quantum dynamics of this wherequantum couplings systems and the role Ω ofis quantum the entanglement Rabi1, and frequency, ena- system is governed ∆ by isthe Hamiltonian a laser detuning and ble realizations and studies of new states of matter, even away from 6 H Ωi i V equilibrium.C r Theseare systems replusive also form the basis of van the realization der of Waals interactions.=−σΔiinV+ ijnnij i;j = 2 ∑∑x ∑ (1) quantum informationi;j processors . Although basic building blocks of ħ i 2 i ij< ∼such processors have been demonstrated in systems of a few coupled 3–5 qubits , the current challenge is to increase the number of coherently where Δi are the detunings of the driving lasers from the Rydberg i coupled qubits to potentially perform tasks that are beyond the reach state (Fig. 1b), σx =|gri〉〈 ii|+|rg〉〈 i| describes the coupling between of modern classical machines. the ground state |gi〉 and the Rydberg state |ri〉 of an atom at position i, Several physical platforms are currently being explored to reach these driven at Rabi frequency Ωi, ni = |ri〉〈ri|, and ħ is the reduced goals. Systems composed of about 10–20 individually controlled atomic Planck constant. Here, we focus on homogeneous coherent coupling ions have been used to create entangled states and to explore quantum (|Ωi| = Ω, Δi = Δ), controlled by changing laser intensities and 6,7 simulations of Ising spin models . Similarly sized systems of pro- detunings in time. The interaction strength Vij is tuned either by grammable superconducting qubits have been implemented recently8. varying the distance between the atoms or by coupling them to a Quantum simulations have been carried out in larger ensembles of different Rydberg state. more than 100 trapped ions without individual readout9. Strongly The experimental protocol that we implement is depicted in Fig. 1c interacting quantum dynamics has been explored using optical lattice (see also Extended Data Fig. 1). First, atoms are loaded from a magneto- simulators10. These systems are already addressing computationally optical trap into a tweezer array created by an acousto-optic deflector. difficult problems in quantum dynamics11 and the fermionic Hubbard We then use a measurement and feedback procedure that eliminates 12 2 model . Larger-scale Ising-like machines have been realized in super- the entropy associated with the probabilistic trap loading and results Seeconducting also13 anotherand optical14 systems, recent but these experiment realizations lack eitherZhang in the rapidet production al. 2017of defect-free claiming arrays with more 53 than qubits50 laser- coherence or quantum nonlinearity, which are essential for achieving cooled atoms, as described previously26. These atoms are prepared full quantum speedup. in a preprogrammed spatial configuration in a well-defined internal ground state |g〉 (Methods). We then turn off the traps and let the Arrays of strongly interacting atoms system evolve under the unitary time evolution U(Ω, Δ, t), which is A promising avenue for realizing strongly interacting quantum matter realized by coupling the atoms to the Rydberg state |r〉 = |70S1/2〉 with involves coherent coupling of neutral atoms to highly excited laser light along the array axis (Fig. 1a). The final states of individual Rydberg states15,16 (Fig. 1a). This results in repulsive van der Waals atoms are detected by turning the traps back on and imaging the recap- 6 interactions (of strength VCij =/Rij) between Rydberg atom pairs at a tured ground-state atoms via atomic fluorescence; the anti-trapped distance Rij (ref. 15), where C > 0 is the van der Waals coefficient. Such Rydberg atoms are ejected. The atomic motion in the absence of traps interactions have recently been used to realize quantum gates17–19, to limits the time window for exploring coherent dynamics. For a typical implement strong photon–photon interactions20 and to study quantum sequence duration of about 1 μs, the probability of atom loss is less than many-body physics of Ising spin systems in optical lattices21–23 and in 1% (see Extended Data Fig. 2). 1Department of Physics, Harvard University, Cambridge, Massachusetts 02138, USA. 2Department of Physics and Research Laboratory of Electronics, Massachusetts Institute of Technology, Cambridge, Massachusetts 02139, USA. 3Institute for Theoretical Atomic, Molecular and Optical Physics, Harvard-Smithsonian Center for Astrophysics, Cambridge, Massachusetts 02138, USA. 4Division of Physics, Mathematics and Astronomy, California Institute of Technology, Pasadena, California 91125, USA. 30 NOVEMBER 2017 | VOL 551 | NATURE | 579 © 2017 Macmillan Publishers Limited, part of Springer Nature. All rights reserved. Quantum revivals I For homogeneous couplings and in the limit Vj;j+1 Ω ∆ periodic quantum revivals were observed. I This is especially surprising considering that the system is non-integrable as 1.0 L = 28 L = 32 0.8 evidenced by the level statistics.2 i | ) t ( 0.6 2 Z | 2 0.4 Z 1.0 | h L = 32 0.2 Poisson 0.0 0.8 Semi-Poisson 0 10 20 30 Wigner-Dyson t ) 0.6 s ( P 0.4 0.2 0.0 0 1 2 3 s An effective model In this same limit the dynamics is generated by an effective Hamiltonian X H = Pj 1Xj Pj+1 (2) − j in an approximation well controlled up to times exponential in Vj;j+1=Ω which reproduces the same phenomena. The Hilbert space of the model acquires a kinematic constraint. Each atom can be either in the ground or the excited state , but configurations where two adjacent atoms|◦i are both excited |•i are forbidden. This makes the Hilbert space similar to thatj · · · •• of · chains · · i of Fibonacci anyons3. 3Feiguin et al. 2007; Lesanovsky and Katsura 2012. From dynamics to eigenvalues 0 L = 32 2 I A band of special states 2 − which account for most of i | ψ 4 | − the N´eel state. 2 Z 6 I These have approximately | h − equally spaced eigenvalues, log 8 − and converging with system 10 size. − 20 10 0 10 20 I Explains the oscillatory − − E dynamics. Goal: Find or otherwise explain these special states. Forward-scattering approximation Split the Hamiltonian H = H+ + H into a forward propagating part − X X H+ = Xj Pj 1Qj Pj+1 + Xj Pj 1Pj Pj+1 (3) − − j even j odd and backward propagating part H = H+y . The forward-propagator increases distance from N´eelstate− by one, and the backward-propagator decreases it. Forward-scattering approximation Build an orthonormal basis for the Krylov subspace generated by H+ starting from the N´eelstate 0 ; 1 ;:::; L . The Hamiltonian projected into this subspacefj i j i is a tight-bindingj ig chain L X HFSA = βn ( n n + 1 + h.c.) (4) j i h j n=0 with hopping amplitudes βn = n + 1 H+ n = n H n + 1 .