⇦Chinese Physics Letters, 2020, Vol. 37, No. 6, Article code 065201 Terahertz Radiation from a Longitudinal Electric Field Biased Femtosecond Filament in Air * Yi Liu (刘一)1**, Shaojie Liu (刘少杰)1, Aurélien Houard2, André Mysyrowicz2, Vladimir T. Tikhonchuk3,4 Affiliations 1Shanghai Key Lab of Modern Optical System, University of Shanghai for Science and Technology, Shanghai 200093, China 2Laboratoire d'Optique Appliquée, ENSTA Paris, Ecole Polytechnique, CNRS, Institut Polytechnique de Paris, 828 Boulevard des Maréchaux, 91762 Palaiseau cedex, France 3Centre Lasers Intenses et Applications, University of Bordeaux-CNRS-CEA, 351 Cours de la Liberation, 33405 Talence cedex, France 4ELI-Beamlines, Institute of Physics, Czech Academy of Sciences, 25241 Dolní Břežany, Czech Republic Received 5 March 2020, online 26 May 2020 *Supported by the National Natural Science Foundation of China (Grant No. 11574213) and the Innovation Program of Shanghai Municipal Education Commission (Grant No. 2017–01-07-00-07-E00007).
**Corresponding author. Email: yi.liu@usst.edu.cn Citation Text: Liu Y, Liu S J, Houard A, Mysyrowicz A and Tikhonchuk V T et al 2020 Chin. Phys. Lett. 37 065201    Abstract The terahertz (THz) temporal waveform and spectrum from a longitudinal electrically biased femtosecond filament is studied experimentally. The initial direction of the electron motion inside the unbiased filament plasma is deduced from the transformation of the THz temporal waveform with applied fields of opposite polarities. Furthermore, a spectrum shift to lower frequency of the THz spectrum is observed in the presence of a biased field. It agrees well with theoretical predictions. DOI:10.1088/0256-307X/37/6/065201 PACS:52.59.Ye, 41.60.-m, 52.25.Os, 52.38.Hb © 2020 Chinese Physics Society Article Text Terahertz radiation from plasma in air induced by laser pulses was first demonstrated by Hamster and co-workers about 25 years ago.[1] In recent years, the THz field from the long plasma channel in a filament generated by an intense femtosecond laser has attracted much attention.[2–12] This air plasma THz source holds several unique advantages compared to traditional technique including photoconductive antenna and optical rectification with optical-electrical crystals. With femtosecond filament, THz sources can be positioned far away from laser systems, bypassing the detrimental absorption of the THz field by water vapor during propagation in ambient air.[13,14] At the same time, high power laser pulses up to several terawatts can be employed for THz generation without damage to the emitter, which is impossible with the traditional techniques.[13] However, the conversion efficiency of this single-color filamentation method has been measured to be low, on the order of 10$^{-9}$.[15,16] Several methods have been demonstrated to enhance the THz field, such as applications of transverse or longitudinal electric field,[4,17,18] bifilamentation technique,[19] and two-color or multiple-color excitation.[2,3,5–12,20–23] In particular, the presence of a longitudinal field can enhance the intensity of low frequency components by 1000 times.[18] Furthermore, the physical properties of THz emission from filaments remain the same as those excited with a single-color femtosecond pulse, including the characteristic radial polarization and hollow cone radiation pattern. It has been attributed to an enhanced transition-Cherenkov (TC) radiation from the filament plasma.[18] In this Letter, we report the characterization of the temporal waveform and spectrum of THz radiation from longitudinally electrical biased filaments. In the previous study, the characterization was performed with a heterodyne detector working at 0.1 THz with a bandwidth of 4 GHz, limiting the insight into the enhanced THz radiation.[18] Here the full temporal form of the THz emission is recorded by electro-optical detection. It is revealed that in the presence of electric fields with opposite polarities, the time domain THz waveform experiences a 180$^{\circ}$ phase shift. From these measurements, the initial direction of the electron motion inside a free filament is inferred to be toward the laser. Furthermore, the THz spectra from filaments with an external field show a spectrum shift towards lower frequency. Both effects are well explained by the theoretical Cerenkov-transition model. In the experiment, a chirped pulse amplification (CPA) femtosecond laser system was employed. This femtosecond laser system delivers 35 fs pulses at 800 nm, with pulse energy up to 8 mJ. The pulses were split into two beams with a 90/10 beam splitter. In our experiment, up to 3 mJ pulses were focused by a 180 mm convex lens to generate a plasma filament in ambient air. The length of the plasma filament varied from 3 to 8 mm, depending on the incident power. Two circular copper electrodes of 40 mm diameter with central holes were mounted on the filament, as presented in Fig. 1. The two electrodes were separated by about 15 mm, with the filament placed around the middle. The diameters of the holes on the two electrodes were 3 and 10 mm, respectively. A larger opening at the exit ensured that the THz field was not blocked by the electrode plate. A static voltage was applied to the exit electrode and the incident electrode was grounded. A high resistance silicon plate was employed to block the fundamental pump pulse after the plasma, while leaving the THz emission to pass through. The THz emission from the biased filaments was first collimated by an off-axis parabolic mirror with focal length of 120 mm. It was then focused with an identical parabolic mirror to a 1-mm-thick (110) ZnTe crystal for electro-optical detection with the weak 800 nm probe.
cpl-37-6-065201-fig1.png
Fig. 1. Schematic diagram of the experimental setup for the electric field biased filaments. The femtosecond laser pulse propagates from the left to the right. A pair of circular electrodes with central holes were mounted on the filament to apply a longitudinal electric field.
cpl-37-6-065201-fig2.png
Fig. 2. Waveforms of the THz field from the biased filaments: (a) no external field, (b)–(e) electric field in the direction of laser propagation, (f)–(j) with electric field in the opposite directions of laser propagation. The applied voltages on the 15 mm separated plate electrodes are indicated in each panel.
In Fig. 2, we present the waveforms of the THz field from the biased filaments as a function of the polarity and strength of the longitudinal electric field. All these THz waveforms are normalized to their maximum for a better view of the details. Therefore, a better signal-to-noise ratio corresponds to a stronger THz field when we compare these waveforms, since the noise level remains constant for all the measurements. We note that the secondary THz peak around $t = 17$ ps correspond to the round-trip of the THz radiation inside the silicon filter due to the surface reflection. In the presence of a negative voltage (electric field in the direction of laser propagation), the THz field increases monotonically from $E_{\rm ex} = 0$ kV/cm with a slight distortion up to $E_{\rm ex} = 9$ kV/cm (Figs. 2(a)–2(e)). In the opposite case (positive voltage), the evolution of the THz waveform is different. First of all, the THz signal decreases with increasing electric field up to $E_{\rm ex} \sim 3$ kV/cm, which is evident from a much smaller SNR in Fig. 2(h) compared to Fig. 2(a). With further increase of the field, the THz starts to increase again. At the same time, a complicated transformation of the THz waveform is noticeable. In the presence of relatively high field ($E_{\rm ex} \ge 4.5$ kV/cm), the THz waveforms finally exhibit an inverse polarity, when compared to positive voltage.
cpl-37-6-065201-fig3.png
Fig. 3. Peak-to-peak amplitude of the THz field as a function of the external electric field. The error bars denote the standard derivation of the measured signal.
The peak-to-peak (PTP) amplitudes of the THz field are presented as a function of the external electric field in Fig. 3. In the presence of weak electric field, the PTP amplitude is not well defined due to the multiple peak structure of the THz field. Here we just pick up the values of the maxima of the positive/negative peaks in relevant cases. We find that the THz amplitude depends on the field strength linearly, which is in agreement with our previous report of quadratic dependence of the THz intensity on electric field strength.[18] A minimum THz signal obtained around $E_{\rm ex} = 1.5$ kV/cm is now evident, suggesting that the spontaneous electric field inside the filament is on the order of $-1.5$ kV/cm. This actually provides a simple experimental method to estimate the spontaneous electric field inside the plasma filament. More important, this observation means that the presence of a positive electric field largely suppresses the spontaneous electron motion inside a free plasma filament, indicating that its initial electron motion is pointed backward with reference to the laser propagation direction. This result is different from that obtained in a previous report, where it was found that electrons inside a N$_{2}$ filament oscillate initially in the laser propagation direction.[24] However, we note that the focusing geometry ($f = 180$ mm) and laser energy (3 mJ) in the present experiment are different from those in Ref. [24] ($f = 1000$ mm, 1 mJ). As discussed in Ref. [24], the initial electron movement direction is determined by a delicate balance between the laser pressure acting in the forward direction and a backward oriented plasma wake force. Therefore, the tighter focusing appears to tilt this balance in favor of a stronger plasma wake force. We note that in the presence of external field the THz field oscillation period increases gradually, by comparing Figs. 2(a) and 2(e). In Fig. 4(a), we present the spectra of the THz radiation with and without the longitudinal field corresponding to the above two waveforms. A spectrum shift towards low frequency is noticeable, in the presence of an external field $E_{\rm ext} = 9$ kV/cm. This suggests that the frequency component of the plasma current induced by the external field is different from that induced by the laser pulse itself. Also, we would like to point out that the spectrum in Fig. 2(j) is almost identical to that of Fig. 2(e), as expected from their similar temporal waveforms.
cpl-37-6-065201-fig4.png
Fig. 4. (a) THz spectrum in the presence of the electric field of $E_{\rm ex} = - 6$ kV/cm (red dashed line) and that without the field (black line). (b) Calculated plasma current spectrum with (red dashed line) and without (black line) the bias electric field.
In the case of plasma filaments without external electric field, the longitudinal ponderomotive force of the rear side of the laser pulse accelerates the newly born electrons. It initializes an electron motion in the backwards direction, and creates an electrostatic field inside the filament in its wake. This charge separation in the longitudinal direction provokes an oscillating current. The Fourier spectrum of the current reads[18,25] $$\begin{align} j_{z}^{w} (\omega)=\,&\frac{e\omega_{\rm pe}^{2} I_{0} }{2m_{\rm e} c^{2}\omega_{0}^{2} }\frac{\omega +2i\nu_{\rm e} }{\omega_{\rm pe}^{2} -\omega^{2}+i\nu_{\rm e} \omega }\frac{\sin ({\omega \tau_{\rm L}} /2)}{1- ({{\omega \tau_{\rm L}} /{2\pi} })^{2}}\\ &\cdot\exp \Big({-\frac{i\omega \tau_{\rm L} }{2}} \Big),~~ \tag {1} \end{align} $$ where $I_{0}$, $\omega_{0}$ and $\nu_{\rm e}$ are the laser intensity, laser frequency and the electron collision frequency, respectively. The current spectrum has a maximum at the electron plasma frequency $\omega_{\rm pe} =\sqrt {{e^{2}n_{\rm e} } / {m_{\rm e} \varepsilon_{0} }}$, and its amplitude is proportional to the laser intensity. The external longitudinal electric field is well below the discharge threshold and it does not affect the ionization process in air driven by the laser pulse. Nevertheless, the external field $E_{\rm ext}$ can easily exceed the wake electric field $E_{\rm w}$ created by the laser ponderomotive force. As a result, the electrons ionized by the laser field are now accelerated by the total longitudinal electric field, $E_{\rm ext} + E_{\rm w}$, originated from the laser ponderomotive force and the external field. The current spectrum due to the external electric field can be expressed by $$ j_{z}^{e} (\omega)=\frac{\varepsilon_{0} \omega_{\rm pe}^{2} E_{\rm ext} }{\omega^{2}-\omega_{\rm pe}^{2} +i\nu_{\rm e} \omega },~~ \tag {2} $$ which depends on the external field $E_{\rm ext}$ linearly.[18] This explains naturally the experimentally observed linear dependence of the THz amplitude on the external field presented in Fig. 3. The absolute value of the current spectra given by Eqs. (1) and (2) are plotted in Fig. 4(b). Good agreement is found with our experimental observation by adopting an electron density of $0.9\times 10^{16}$ cm$^{-3}$ and a collision frequency of $v_{\rm e} = 0.35$ THz, which are typical values for the plasma filaments formed in ambient air.[26,27] Qualitatively speaking, the spectra in Eqs. (1) and (2) are different because the laser ponderomotive force is of a short duration ($\sim $40 fs) thus giving additional $\omega$ in the numerator in Eq. (1). Contrarily, the external field is static, its Fourier transformation gives 1/$\omega$ in the spectrum thus downshifting the spectrum. In conclusion, we have measured the THz waveform from femtosecond filaments, which is longitudinally biased with an external electrical field. A complicated THz waveform distortion is observed in the presence of relatively weak electric field ($E_{\rm ex} < 4.5$ kV/cm). A minimum THz signal is observed with electric field in the opposite direction of laser propagation with strength of $E_{\rm ex} = 1.5$ kV/cm, suggesting that the pondermotive force induces electron motion inside a field free plasma filament in the backward direction of laser propagation. We further compare the THz spectrum from the filaments with and without the external field. A spectrum shift towards a lower frequency is observed in the presence of the field, which is well explained by a theoretical model. References Subpicosecond, electromagnetic pulses from intense laser-plasma interactionIntense terahertz pulses by four-wave rectification in airCoherent control of terahertz supercontinuum generation in ultrafast laser–gas interactionsGeneration of terahertz pulses by photoionization of electrically biased airCoherent Polarization Control of Terahertz Waves Generated from Two-Color Laser-Induced Gas PlasmaBroadband terahertz wave remote sensing using coherent manipulation of fluorescence from asymmetrically ionized gases3D Numerical Simulations of THz Generation by Two-Color Laser FilamentsUltrabroad Terahertz Spectrum Generation from an Air-Based Filament PlasmaManipulation of polarizations for broadband terahertz waves emitted from laser plasma filamentsHighly enhanced terahertz conversion by two-color laser filamentation at low gas pressuresObservation of Terahertz Radiation via the Two-Color Laser Scheme with Uncommon Frequency RatiosModulation of terahertz generation in dual-color filaments by an external electric field and preformed plasmaConical Forward THz Emission from Femtosecond-Laser-Beam Filamentation in AirRemote generation of high-energy terahertz pulses from two-color femtosecond laser filamentation in airHigh current permanent discharges in air induced by femtosecond laser filamentationBroadband THz emission from gas plasmas induced by femtosecond optical pulses: From fundamentals to applicationsStrong Enhancement of Terahertz Radiation from Laser Filaments in Air by a Static Electric FieldAmplification of transition-Cherenkov terahertz radiation of femtosecond filament in airTerahertz Radiation Source in Air Based on Bifilamentation of Femtosecond Laser PulsesBoosting Terahertz Generation in Laser-Field Ionized Gases Using a Sawtooth Wave ShapeTerahertz radiation generation by three-color laser pulses in air filamentModulation of terahertz-spectrum generation from an air plasma by tunable three-color laser pulsesStrong terahertz radiation from air plasmas generated by an aperture-limited Gaussian pump laser beamMeasurement and Control of Plasma Oscillations in Femtosecond FilamentsForward THz radiation emission by femtosecond filamentation in gases: theory and experimentFemtosecond filamentation in transparent mediaThe propagation of powerful femtosecond laser pulses in opticalmedia: physics, applications, and new challenges
[1] Hamster H, Sullivan A, Gordon S, White W and Falcone R W 1993 Phys. Rev. Lett. 71 2725
[2] Cook D J and Hochstrasser R M 2000 Opt. Lett. 25 1210
[3] Kim K Y, Talor A J, Glownia J H and Rordriguez G 2008 Nat. Photon. 2 605
[4] Löffler T, Jacob F and Roskos H G 2000 Appl. Phys. Lett. 77 453
[5] Dai J, Karpowicz N and Zhang X C 2009 Phys. Rev. Lett. 103 023001
[6] Liu J, Dai J, Chin S L and Zhang X C 2010 Nat. Photon. 4 627
[7] Berge L, Skupin S, Kohler C, Babuchkin I and Herrmann J 2013 Phys. Rev. Lett. 110 073901
[8] Andreeva V A, Kosareva O G, Panov N A, Shipilo D E, Solyankin P M, Esaulkov M N, González de Alaiza Martinez P, Shkurinov A P, Makarov V A, Bergé L and Chin S L 2016 Phys. Rev. Lett. 116 063902
[9] Zhang Z, Chen Y, Cui S, He F, Chen M, Zhang Z, Yu J, Chen L, Sheng Z and Zhang J 2018 Nat. Photon. 12 554
[10] Yoo Y J, Jang D and Kim K Y 2019 Opt. Express 27 22663
[11] Zhang L, Wang W, Wu T, Zhang R, Zhang S, Zhang C, Zhang Y, Sheng Z and Zhang X C 2017 Phys. Rev. Lett. 119 235001
[12] Li M, Li A Y, He B Q, Yuan S and Zeng H P 2016 Chin. Phys. B 25 044209
[13] D'Amico C, Houard A, Franco M, Prade B, Mysyrowicz A, Couairon A and Tikhonchuk V T 2007 Phys. Rev. Lett. 98 235002
[14] Wang T J, Daigle J F, Yuan S, Theberge F, Chateauneuf M, Dubois J, Roy G, Zeng H and Chin S L 2011 Phys. Rev. A 83 053801
[15] Houard A, Liu Y, Mysyrowicz A and Leriche B 2007 Appl. Phys. Lett. 90 171501
[16] Thomson M D, Kre M, Löffler T and Roskos H G 2007 Laser & Photon. Rev. 1 349
[17] Houard A, Liu Y, Prade B, Tikhonchuk V and Mysyrowicz A 2008 Phys. Rev. Lett. 100 255006
[18] Liu Y, Houard A, Prade B, Mysyrowicz A, Diaw A and Tikhonchuck V 2008 Appl. Phys. Lett. 93 051108
[19] Liu Y, Houard A, Prade B, Akturk S, Mysyrowicz A and Tikhonchuk V 2007 Phys. Rev. Lett. 99 135002
[20] Martinez P G, Babushkin I, Bergé L, Skupin S, Cabrera-Granado E, Kohler C, Morgner U, Husakou A and Herrmann J 2015 Phys. Rev. Lett. 114 183901
[21] Vaičaitis V, Balachninaitė O, Morgner U and Babushkin I 2019 J. Appl. Phys. 125 173103
[22] Lu C, Zhang C, Zhang L, Wang X and Zhang S 2017 Phys. Rev. A 96 053402
[23] Peng X Y, Li C, Chen M, Toncian T, Jung R, Willi O, Li Y T, Wang W M, Wang S J, Liu F, Pukhov A, Sheng Z M and Zhang J 2009 Appl. Phys. Lett. 94 101502
[24] Zhou B, Houard A, Liu Y, Prade B, Mysyrowicz A, Couairion A, Mora P, Smeenk C, Arissian L and Corkum P 2011 Phys. Rev. Lett. 106 255002
[25] Amico C D, Houard A, Akturk S, Liu Y, Bloas J L, Franco M, Prade B, Couairon A, Tikhonchuk V T and Mysyrowicz A 2008 New J. Phys. 10 013015
[26] Couairon A and Mysyrowicz A 2007 Phys. Rep. 441 47
[27] Chin S L, Hosseini S A, Liu W, Luo Q, Théberge F, Aközbek N, Becker A, Kandidov V P, Kosareva O G and Schroder H 2005 Can. J. Phys. 83 863