Abstract
Instabilities are common phenomena frequently observed in nature, sometimes leading to unexpected catastrophes and disasters in seemingly normal conditions. One prominent form of instability in a distributed system is its response to a harmonic modulation. Such instability has special names in various branches of physics and is generally known as modulation instability (MI). The MI leads to a growthdecay cycle of unstable waves and is therefore related to FermiPastaUlam (FPU) recurrence since breather solutions of the nonlinear Schrödinger equation (NLSE) are known to accurately describe growth and decay of modulationally unstable waves in conservative systems. Here, we report theoretical, numerical and experimental evidence of the effect of dissipation on FPU cycles in a super wave tank, namely their shift in a determined order. In showing that ideal NLSE breather solutions can describe such dissipative nonlinear dynamics, our results may impact the interpretation of a wide range of new physics scenarios.
Introduction
The discovery of the FermiPastaUlam (FPU) recurrence was a significant step in nonlinear dynamics. It describes the natural return cycle of a dynamical system to its initial conditions after undergoing complex motion dynamics^{1,2}. Meanwhile, the FPU recurrence has been studied and observed in several nonlinear media. For instance, in hydrodynamics within the framework of the Korteweg De Vries^{3} equations as well as in a more broad range in physics within the context of the nonlinear Schrödinger equation (NLSE)^{4,5}, particularly, in the description of modulationally unstable periodic packets returning to the initial state of small perturbation of the background after significant envelope compression^{6,7}.
In fact, the NLSE admits an analytic family of timeperiodic solutions, referred to as Akhmediev breathers (ABs), which describe the dynamics of the modulation instability (MI) in time and space. ABs describe the MI starting from a regular background, significantly enhancing waves’ amplitudes during the envelope compression until reaching a specific saturation point and finally declining the envelope back to the regular state. The use of breathers such as ABs in the study of MI is very convenient from an experimental view point, since the MI becomes therefore initiated at any growth rate stage. Note that triggering the MI in the spectral domain, starting from small sideband amplitudes, may require a significant propagation distance and time for the observation of one compression cycle^{8,9}.
However, when performing laboratory experiments deviation from expected AB trajectories in the phase space are expected, since medium properties are never perfectly described through the coefficients of the NLSE approximation. Indeed, these deviations, which are due to the medium’s properties and imperfect laboratory environments, lead to the observation of recurrent MI growthdecay cycles. In fiber optics, experimental observations of the FPU recurrence within the framework of MI have been also restricted to only one whole cycle^{10,11}. More recently, the effects of different perturbations to the standard NLSE such as thirdorder dispersion or varying dispersion, or even the impact of initial excitation of MI, on the FPU phenomenon have been reported as well in refs 12, 13, 14, 15. Furthermore, similar physical properties in other evolution equation have been discussed in ref. 16.
Besides higherorder dispersive effects as well as nonlinearities, one possible physical action that causes deviations from expected NLSE dynamics is the presence of dissipation in the medium. For water waves, the impact of dissipation on swell propagation and on MI has been studied and discussed in refs 17,18. In these interesting studies, it has been shown that strong dissipation may inhibit the occurrence of MI or exhibiting a significant downshifting. As shall be described, the dissipation rates in our work is very small, compared to the rates discussed in the latter studies. Therefore, neither obstruction of MI nor downshifting has be been observed. We also rather address the effect of dissipation on the FPU recurrence cycles.
Here, we show theoretically, numerically and experimentally that the impact of weak dissipation engenders shifted FPU recurrence in the localizations of periodic breathers up to two and a half recurrence cycles. The experimental results, which have been performed in a super water wave tank, are in very good agreement with corresponding numerical NLSE simulations. Due to the interdisciplinary character of the approach, this study may emphasize a wide range of applications in other nonlinear dispersive media, as will be discussed.
Results
The variety of periodic pulsating envelopes
The NLSE is a significant evolution equation used in wave in physics. It describes waves on the surface of the ocean, pulses in optical fibers, special states of BoseEinstein condensates, plasma oscillations and many other phenomena. The NLSE can be written in dimensionless form as
Here, ξ describes the spatial coordinate, moving with the group velocity, while τ denotes the scaled time and ψ the scaled envelope amplitude. Among elementary solutions of the NLSE are plane waves, solitons, breathers and rational solutions^{19}. Breathers can be considered as heteroclinic orbits connecting two saddle points in an infinitedimensional phase space. The latter are plane wave solutions that are modulationally unstable. Saddle points are usually surrounded by nearby trajectories that are connected to similar trajectories around the second saddle point. As a result, homoclinic orbits are surrounded by the periodic trajectories and corresponding solutions of the NLSE^{20}. One of such periodic solution of the NLSE has the form
where
and κ is a free parameter of this family of solutions. Note that this solution is periodic in both τ and ξ with periods defined by κ. In the limit κ → 1, it reduces to the AB solution that exhibits largest gain^{20}
which has infinite the period in ξ and which is the above mentioned homoclinic orbit. On the other hand, in the limit κ → 0, period in τ becomes infinite and it converges to the wellknown basic bright soliton solution:
The periodic solution that is located on the other side of the homoclinic orbit (or separatrix) reads
Here, the second argument in the Jacobi elliptic functions corresponds to the elliptic modulus, rather than the elliptic parameter m = k^{2}. Two examples of each periodic solution with respect to (2) for κ = 0.7 and (6) for k = 0.8 are shown in Fig. 1.
The solution (6) can be alternatively derived from the solution (2) taking κ > 1 and using the transformations for elliptic Jacobi functions for the case κ = 1/k. Details can be found in ref. 21. As k → 1, the solution (6) has formula (4) as its limit. As solutions (6) and (2) are located on different sides of the separatrix (4) they are qualitatively different. The solution (2) keeps maxima of the periodic function at the same position while the solution (6) has maxima alternating. The latter can be considered as phaseshifting solutions. This difference can be seen clearly in Fig. 1.
The geometric interpretation of two types of periodic solutions is presented in Fig. 2. The circle with unit radius shown by the dashed line can be considered as a plane wave with unit amplitude and variable phase. Each point of the circle is an unstable saddle point. The starting trajectories of the saddle point describe the BenjaminFeir or the MI. Let us choose one of them located, say, at the upper point of the circle. Continuation of the trajectory that starts at the saddle point ends up at another saddle point located at the bottom of the circle. This particular trajectory describes the Akhmediev breather (4). This trajectory is a heteroclinic orbit separating two trajectories denoted as A and B corresponding to the periodic solutions (6) and (2). Trajectory A rotates on one side of the complex plane and does not shift the phase while trajectory B rotates around the origin thus gaining the phase difference 2π on each period of oscillations.
FermiPastaUlam recurrence and breathers in the presence of dissipation
These two types of solutions can be observed in experiments that start with MI. In the presence of even small perturbations, the separatrix may be converted into a nearby periodic orbit of either type A or type B depending on the sign of the perturbation. In the hydrodynamic experiments that are described in the present work, the dissipation played the role of the perturbation. The main source of dissipation is the friction with the walls of the tank and the friction with air. An interesting point here is the fact that despite the dissipation always has the same sign, the perturbation it causes can be either positive or negative. Consequently, the trajectory could be converted either to type A or type B during the evolution. These two scenarios can be easily detected experimentally observing the phase shift. Note that one possible shifting form of ABs has been experimentally studied in ref. 22. However, the shifting discussed here has another physical origin and evolution.
We confirm the occurrence of this interesting phenomenon in numerical simulations and validate the results through hydrodynamic laboratory experiments conducted in a large wave facility permitting the measurement of several stages of envelope compressions. Namely, we reveal that deviations from exact AB envelope dynamics caused by nonideal excitation or propagation losses imply the emergence of successive spatial recurrences as shown in Fig. 1. In particular, the specific phaseshift of the envelope modulation cycles caused by dissipation is observed experimentally.
The solutions given above are related to the MI with the highest growth rate. In this particular case, the phase shift of one growthdecay cycle is equal to π. Any other frequency within the instability band produces its own phase shift which varies from zero to 2π. The whole family of Akhmediev breathers (ABs)^{20} is given by
where and . Here while Ω and R determine the modulation frequency and corresponding growth or decay rate near the saddle point, respectively. Note that Eq. (4) is a particular case of the AB solutions (7). When the solution describes the MI in the event of maximal growth rate. When , the same solution describes the family of space periodic KuznetsovMa breathers^{23,24}. In the limiting case of , the growth rate becomes algebraic and the solution reduces to a rational doublylocalized solution, known as the Peregrine solution^{25}. The latter breather solutions attracted scientific interest recently^{26,27} and had been observed in several nonlinear systems^{11,28,29,30,31,32}. Solutions (7) are of significant importance in understanding the MI as well as for a wide range of applications, since they exactly and physically describe the complete growth  decay cycle of MI, quantifying in detail the sideband triangularcomb cascade dynamics^{13,33}.
Figure 3(a) shows an example of exact AB evolution for the breather parameter , while Fig. 3(b) shows the trajectory on the complex plane that corresponds to this evolution. The total phase shift provided by this trajectory is higher than π which means that the MI frequency is detuned from the highest growth rate regime.
Indeed, small perturbation of the initial conditions causes the recurrent breathing of AB envelopes. The trajectory misses the exact saddle point and continues along the hyperbolic orbit. This results in the next recurrent dynamics which then continues into periodic motion^{13}. An example of two successive recurrences is depicted in Fig. 3(c) when approximate initial conditions are used in the numerical NLSE simulations. Here, the theoretical AB profile at ξ = −2.5 was fitted by a simple cosine modulation of the background wave with same frequency and amplitude.
In physical systems deviations from exact conditions may be caused by several sources, such as higherorder dispersion and inelastic Raman scattering in optical fibers^{34} or the mean flow of Stokes waves in hydrodynamics^{35}. Another example is the effect of weak dissipation. The latter shifts the wave profile from the exact shape leading the trajectory to miss the saddle point. The model describing the weak attenuation of the wave envelope is the NLSE with dissipation^{36}:
where is the normalized attenuation rate. The effect of linear attenuation on the AB dynamics in particular can now be studied numerically. As we will see next, the effect of the dissipation will originate a π/2 phaseshift in the recurrent breather compression. Figure 4(a,c,e) shows the corresponding impact on the AB evolution using exact initial conditions, determined by , while the dissipation rate is varied as , respectively.
This is a remarkable phenomenon, which we will refer to as phaseshifted FPU recurrence. Note that this latter particular recurrence would also occur in the case of cosine modulated Stokes background in the presence of dissipation. As experiments related to MI are more accurately designed in the time space domain within the framework of breathers, we decided to use ABs to initiate the wave motion for the laboratory experiments. Furthermore, the dissipation rate is responsible for shifted cycle periods for all modulation frequencies. When the modulation frequency tends to zero (Peregrine breather case^{25}), experimental observations of the phaseshifted FPU recurrence would be more ambiguous. Moreover, the higher the dissipation rate, the faster orbit deviations occur and the shorter the recurrence cycles.
Experimental setup
Experiments have been performed in a super tank, installed at the Tainan Hydraulics Laboratory (THL) of National Cheng Kung University in Taiwan. The facility is 200 m long, 2 m wide and 2 m high. The water depth was set to 1.35 m. The tank is equipped with a piston wavemaker, which generates the waves at one end of the flume, while an absorbing beach is installed at the other end. In order to measure wave elevation, 60 capacitancetype wave gauges, with a sample rate of 100 Hz, have been deployed along the tank and calibrated accordingly, before conducting the experiments. The first gauge was fixed at 2.1 m from the wavemaker, while the last at 176.1 m. A schematic illustration of the facility is shown in Fig. 5.
Experimental results
Before starting experiments to study the influence of the dissipation on hydrodynamic ABs, we determine the corresponding dissipation rate, obviously always naturally existing, when performing experiments in a narrow and onedimensional water wave basin, in particular, in a significantly long facility. Indeed, there are a number of sources of energy dissipation of waves, such as friction with the walls, friction with air as well as molecular viscosity. The latter becomes important at small scales, especially in the capillary regime (wave of the order of a few centimetres or less). It has been shown in the past that dissipation can be accounted by adding a linear damping term in the NLS equation, see for instance^{37}. For wave tank experiments, where friction with walls cannot be neglected, the damping coefficient is usually obtained experimentally. In the present case, the normalised coefficient is given by the damping coefficient normalised by the dimensional dispersive coefficient in the NLS equation. In order to determine the coefficient we first generate a regular wave train and measured the attenuation of the wave amplitude during its propagation along the flume. For a regular wave field of amplitude a = 0.011 m and steepness ε = ak = 0.09, where k denotes the wave number, the linear dissipation rate was found to be . This corresponds to a wave amplitude attenuation of 23% over a propagation distance in the flume of 155 m. We now use the same parameters for the carrier in order to excite ABs on the corresponding background and set the breather parameter to be . The boundary conditions applied to the wave maker, is determined by the dimensional form of the surface elevation, modelled by the AB. We refer to Methods section for the description of the dimensional transformations, the surface elevation as well as for the assignment of the dissipation rate. The collected temporal surface elevations are then aligned by the value of the group velocity c_{g} for comparison with numerical simulations. Due to the steepness of the background wave train, a nonlinear correction of the group velocity has been taken into account. The envelope of the measured wave trains are then extracted by use of the Hilbert transform and aligned by the value of the group velocity (see i.a. Methods). Figure 6(a) shows the results.
Clearly, the breather recurrent cycles can be observed in excellent agreement with numerical simulations, depicted in Fig. 6(b). This proves the orbit jump^{38,39}, as shown in Fig. 4. In order to confirm the influence of dissipation in engendering recurrent shifted localized envelopes, we performed another set of experiments, however, for different carrier and AB parameters, respectively. In the following we set the amplitude to be a = 0.020 m, the steepness to be ε = 0.11 and the AB parameter , while the dissipation rate is in this case This corresponds to a wave amplitude attenuation of 19% over a propagation distance in the flume of 155 m. All these chosen parameters are beyond breaking thresholds of the unstable waves, and the parameter is below the threshold of higherorder MI^{12}. The evolution of the wave envelope is shown in Fig. 7(a). The corresponding numerical damped NLSE simulations are once again in very good agreement, see Fig. 7(b). Again, we can here clearly observe the π/2phase shift in each FPU recurrence cycle of envelope compression. In both cases, numerical simulations are indeed in strong agreement in matching the modulation period, the recurrence period and the recurrent breather’s strong compressions.
Discussion
We have shown that weak dissipation may initiate specific phaseshifted cycles of π/2 in the evolution of periodic modulationally unstable waves, described by AB. In fact, we discussed the effect of dissipation on the orbit jumps in the complex phase space. The numerical results starting from exact AB initial conditions have been validated by laboratory experiments, conducted in a super tank for different set of breather and background parameters. We predict that this novel phenomena, we refer to as phaseshifted FPU recurrence, will motivate a wide range of applications, due to the multidisciplinary nature of the problem, since the NLSE, accurately models the dynamics of hydrodynamic, electromagnetic as well as plasma waves.
The principally novel aspect of our work is the experimentally observed slip from heteroclinic orbit (breather) to closely located periodic orbits due to the presence of dissipation. Periodic orbits have finite periods in contrast to heteroclinic orbits that have infinite periods. This is caused by the shift of trajectory from exponential one to hyperbolic near the saddle point in Fig. 2. Specifically, the ξperiods of the solutions (2) and (6) are finite and strongly depend on the amount of the shift from the heteroclinic orbit (4). The recurrence cycle then experiences dramatic change from infinite evolution to periodic motion when losses cause such shift.
We emphasize that the observation of many breathing cycles is a very challenging task, in particular to study the effect of perturbations on FPU recurrence without the impact of propagation losses. Indeed, overcoming experimental restrictions in hydrodynamics, such as the dissipation or the nonlinear length to name a few, is not something obvious, even for other physical systems. Varying the parameters of the carrier may enhance the number of recurrence shifted cycles that can be observed. However, increasing the carrier steepness may engender breaking of the waves. Another parameter that controls the period of the cycle, as shown in Fig. 4 is the dissipation rate. For the chosen wave parameters, this value for dissipation cannot be varied in the current experimental setup. For instance, breather waves have also been intensively studied in optical fibers, but limited to one whole cycle of recurrence. This can be simply related to the typical normalized dissipation rate estimated about 3.8 × 10^{−2} (for typical parameters SMF28 optical fiber and 1W continuous wave power^{11,12,32}). This clearly points out both the extreme importance of the hydrodynamic results reported here and capabilities of the super wave tanks compared to nonlinear optics. To go beyond the frontier in terms of testing nonlinear wave theory, it clearly requires to overcome the current limitations of real physical systems.
Methods
Towards experimental initials conditions
The evolution of onedimensional deepwater packets Ψ(x, t), propagating in physical space with the group velocity can be modeled by the deepwater NLSE^{5}
Here, g is the gravitational acceleration and γ the dissipation rate. The wave number and the wave frequency are connected through the linear dispersion relation ω^{2} = gk. The group velocity is then equal to .
The experiments have been conducted in deepwater conditions. Considering the depth being h = 1.35 m, the parameters of the carrier wave have been chosen accordingly. Once the amplitude a and the steepness ε = ak being fixed, the wave frequency can be derived from the dispersion relation for deepwater. In the next step, the AB solution (7) from the scaled NLSE (1) have to be transformed accordingly by setting , and . Then, the non dimensional form of the NLSE is given by
where .
After fixing the breather parameter the Akhmedievtype surface elevation is then given by
The boundary condition of an Akhmediev breather, applied to the wave maker in order to start the evolution of this solution, is determined by evaluating Eq. (11) at a specific position x^{*} of interest.
Reconstruction of the wave envelope evolution
Wave gauges measurements collect the temporal evolution of the water surface, propagating along the wave flume. The temporal variation of envelope Ψ(x^{*}, t) can be reconstructed from a surface measurement η(x^{*}, t), by use of the Hilbert transform H as the following
Figures 6(a) and 7(a) show the whole temporal evolution of the wave envelope, while evolving in space. The latter have been obtained by first aligning the measurements by the group velocity c_{g} = ∂ω/∂k which is deduced from the nonlinear relation dispersion given up to the thirdorder ω^{2} = gk(1 + ε^{2}). After calculating the corresponding complex envelopes by means of the Hilbert transformation, an interpolation has been applied accordingly.
Assessing the dissipation rate
In order to determine the dissipation rate , that in our framework should satisfy
a regular wave train with fixed amplitude and steepness of interest is first generated. The attenuation rate AR in % is then determined from the decay of the latter regular wave train by
Additional Information
How to cite this article: Kimmoun, O. et al. Modulation Instability and PhaseShifted FermiPastaUlam Recurrence. Sci. Rep. 6, 28516; doi: 10.1038/srep28516 (2016).
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Acknowledgements
O.K. acknowledges support from the frenchTaiwanese ORCHID program of the Hubert Curien Partnership (PHC). M.O. was supported by MIUR grant no. PRIN 2012BFNWZ2. M.O. thanks Dr. B. Giulinico for fruitful discussions. B.K. and A.C. acknowledge support from the Burgundy Region (PARI Photcom). A.C. acknowledges support from The Association of German Engineers (VDI) and the Japan Society for the Promotion of Science (JSPS). H.C.H. acknowledges the grant support from MOST 1042628E006014MY3, 1052923E006002MY3 and 1052611I006301.
Author information
Affiliations
AixMarseille University, CNRS, Centrale Marseille, IRPHE, Marseille, France
 O. Kimmoun
 , H. Branger
 & C. Kharif
Tainan Hydraulics Laboratory, National Cheng Kung University, Taiwan
 H. C. Hsu
 , M. S. Li
 & Y. Y. Chen
Dipartimento di Fisica Generale, Universita degli Studi di Torino, Torino, Italy
 M. Onorato
Femtosecond Optics Group, Department of Physics, Imperial College London, London, UK
 E. J. R. Kelleher
Laboratoire Interdisciplinaire Carnot de Bourgogne, UMR 6303 CNRS UBFC, Dijon, France
 B. Kibler
Optical Sciences Group, Research School of Physics and Engineering, Institute of Advanced Studies, The Australian National University, Canberra ACT 020, Australia
 N. Akhmediev
Department of Ocean Technology Policy and Environment, Graduate School of Frontier Sciences, The University of Tokyo, Kashiwa, Chiba 2778563, Japan
 A. Chabchoub
Department of Mechanical Engineering, Aalto University, 02150 Espoo, Finland
 A. Chabchoub
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Contributions
O.K., H.B., M.S.L. and A.C. designed and performed the experiments. B.K., N.A. and A.C. identified the phenomena. The development of the theoretical tool was carried out by H.C.H., Y.Y.C., C.K., M.O., E.J.R.K. and N.A. Numerical simulations have been performed by O.K., B.K. and A.C. All the authors participated in the analysis, interpretation and the writing of the manuscript.
Competing interests
The authors declare no competing financial interests.
Corresponding author
Correspondence to O. Kimmoun.
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Further reading

1.
The Permanent Downshifting at Later Stages of Benjamin–Feir Instability of Waves
Pure and Applied Geophysics (2018)

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Shining light on an old problem
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Fibre multiwave mixing combs reveal the broken symmetry of Fermi–Pasta–Ulam recurrence
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Experiments on higherorder and degenerate Akhmediev breathertype rogue water waves
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